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theoretical physics Theoretical physics is a branch of physics that employs mathematical models and abstractions of physical objects and systems to rationalize, explain and predict natural phenomena. This is in contrast to experimental physics, which uses experimen ...
, a Feynman diagram is a pictorial representation of the mathematical expressions describing the behavior and interaction of
subatomic particle In physical sciences, a subatomic particle is a particle that composes an atom. According to the Standard Model of particle physics, a subatomic particle can be either a composite particle, which is composed of other particles (for example, a prot ...
s. The scheme is named after American physicist
Richard Feynman Richard Phillips Feynman (; May 11, 1918 – February 15, 1988) was an American theoretical physicist, known for his work in the path integral formulation of quantum mechanics, the theory of quantum electrodynamics, the physics of the superfl ...
, who introduced the diagrams in 1948. The interaction of subatomic particles can be complex and difficult to understand; Feynman diagrams give a simple visualization of what would otherwise be an arcane and abstract formula. According to
David Kaiser David I. Kaiser is an American physicist and historian of science. He is Germeshausen Professor of the History of Science at the Massachusetts Institute of Technology (MIT), head of its Science, Technology, and Society program, and a full profess ...
, "Since the middle of the 20th century, theoretical physicists have increasingly turned to this tool to help them undertake critical calculations. Feynman diagrams have revolutionized nearly every aspect of theoretical physics." While the diagrams are applied primarily to
quantum field theory In theoretical physics, quantum field theory (QFT) is a theoretical framework that combines classical field theory, special relativity, and quantum mechanics. QFT is used in particle physics to construct physical models of subatomic particles and ...
, they can also be used in other fields, such as solid-state theory.
Frank Wilczek Frank Anthony Wilczek (; born May 15, 1951) is an American theoretical physicist, mathematician and Nobel laureate. He is currently the Herman Feshbach Professor of Physics at the Massachusetts Institute of Technology (MIT), Founding Direct ...
wrote that the calculations that won him the 2004
Nobel Prize in Physics ) , image = Nobel Prize.png , alt = A golden medallion with an embossed image of a bearded man facing left in profile. To the left of the man is the text "ALFR•" then "NOBEL", and on the right, the text (smaller) "NAT•" then " ...
"would have been literally unthinkable without Feynman diagrams, as would ilczek'scalculations that established a route to production and observation of the
Higgs particle The Higgs boson, sometimes called the Higgs particle, is an elementary particle in the Standard Model of particle physics produced by the quantum excitation of the Higgs field, one of the fields in particle physics theory. In the Standa ...
." Feynman used
Ernst Stueckelberg Ernst Carl Gerlach Stueckelberg (baptised as Johann Melchior Ernst Karl Gerlach Stückelberg, full name after 1911: Baron Ernst Carl Gerlach Stueckelberg von Breidenbach zu Breidenstein und Melsbach; 1 February 1905 – 4 September 1984) was a S ...
's interpretation of the
positron The positron or antielectron is the antiparticle or the antimatter counterpart of the electron. It has an electric charge of +1 '' e'', a spin of 1/2 (the same as the electron), and the same mass as an electron. When a positron collides ...
as if it were an
electron The electron ( or ) is a subatomic particle with a negative one elementary electric charge. Electrons belong to the first generation of the lepton particle family, and are generally thought to be elementary particles because they have no kno ...
moving backward in time. Thus,
antiparticle In particle physics, every type of particle is associated with an antiparticle with the same mass but with opposite physical charges (such as electric charge). For example, the antiparticle of the electron is the positron (also known as an antie ...
s are represented as moving backward along the time axis in Feynman diagrams. The calculation of
probability amplitude In quantum mechanics, a probability amplitude is a complex number used for describing the behaviour of systems. The modulus squared of this quantity represents a probability density. Probability amplitudes provide a relationship between the qua ...
s in theoretical particle physics requires the use of rather large and complicated
integral In mathematics, an integral assigns numbers to functions in a way that describes displacement, area, volume, and other concepts that arise by combining infinitesimal data. The process of finding integrals is called integration. Along with ...
s over a large number of variables. Feynman diagrams can represent these integrals graphically. A Feynman diagram is a graphical representation of a
perturbative In quantum mechanics, perturbation theory is a set of approximation schemes directly related to mathematical perturbation for describing a complicated quantum system in terms of a simpler one. The idea is to start with a simple system for whic ...
contribution to the transition amplitude or correlation function of a quantum mechanical or statistical field theory. Within the
canonical The adjective canonical is applied in many contexts to mean "according to the canon" the standard, rule or primary source that is accepted as authoritative for the body of knowledge or literature in that context. In mathematics, "canonical exampl ...
formulation of quantum field theory, a Feynman diagram represents a term in the Wick's expansion of the perturbative -matrix. Alternatively, the
path integral formulation The path integral formulation is a description in quantum mechanics that generalizes the action principle of classical mechanics. It replaces the classical notion of a single, unique classical trajectory for a system with a sum, or functional ...
of quantum field theory represents the transition amplitude as a weighted sum of all possible histories of the system from the initial to the final state, in terms of either particles or fields. The transition amplitude is then given as the matrix element of the -matrix between the initial and final states of the quantum system.


Motivation and history

When calculating
scattering cross-section In physics, the cross section is a measure of the probability that a specific process will take place when some kind of radiant excitation (e.g. a particle beam, sound wave, light, or an X-ray) intersects a localized phenomenon (e.g. a particle o ...
s in
particle physics Particle physics or high energy physics is the study of fundamental particles and forces that constitute matter and radiation. The fundamental particles in the universe are classified in the Standard Model as fermions (matter particles) and b ...
, the interaction between particles can be described by starting from a
free field In physics a free field is a field without interactions, which is described by the terms of motion and mass. Description In classical physics, a free field is a field whose equations of motion are given by linear partial differential equati ...
that describes the incoming and outgoing particles, and including an interaction
Hamiltonian Hamiltonian may refer to: * Hamiltonian mechanics, a function that represents the total energy of a system * Hamiltonian (quantum mechanics), an operator corresponding to the total energy of that system ** Dyall Hamiltonian, a modified Hamiltonian ...
to describe how the particles deflect one another. The amplitude for scattering is the sum of each possible interaction history over all possible intermediate particle states. The number of times the interaction Hamiltonian acts is the order of the perturbation expansion, and the time-dependent perturbation theory for fields is known as the
Dyson series In scattering theory, a part of mathematical physics, the Dyson series, formulated by Freeman Dyson, is a perturbative expansion of the time evolution operator in the interaction picture. Each term can be represented by a sum of Feynman diagrams ...
. When the intermediate states at intermediate times are energy
eigenstates In quantum physics, a quantum state is a mathematical entity that provides a probability distribution for the outcomes of each possible measurement on a system. Knowledge of the quantum state together with the rules for the system's evolution in t ...
(collections of particles with a definite momentum) the series is called old-fashioned perturbation theory (or time-dependent/time-ordered perturbation theory). The Dyson series can be alternatively rewritten as a sum over Feynman diagrams, where at each vertex both the
energy In physics, energy (from Ancient Greek: ἐνέργεια, ''enérgeia'', “activity”) is the quantitative property that is transferred to a body or to a physical system, recognizable in the performance of work and in the form of heat ...
and
momentum In Newtonian mechanics, momentum (more specifically linear momentum or translational momentum) is the product of the mass and velocity of an object. It is a vector quantity, possessing a magnitude and a direction. If is an object's mass and ...
are conserved, but where the length of the energy-momentum four-vector is not necessarily equal to the mass, i.e. the intermediate particles are so-called off-shell. The Feynman diagrams are much easier to keep track of than "old-fashioned" terms, because the old-fashioned way treats the particle and antiparticle contributions as separate. Each Feynman diagram is the sum of exponentially many old-fashioned terms, because each internal line can separately represent either a particle or an antiparticle. In a non-relativistic theory, there are no antiparticles and there is no doubling, so each Feynman diagram includes only one term. Feynman gave a prescription for calculating the amplitude ( the Feynman rules, below) for any given diagram from a field theory Lagrangian. Each internal line corresponds to a factor of the
virtual particle A virtual particle is a theoretical transient particle that exhibits some of the characteristics of an ordinary particle, while having its existence limited by the uncertainty principle. The concept of virtual particles arises in the perturbat ...
's
propagator In quantum mechanics and quantum field theory, the propagator is a function that specifies the probability amplitude for a particle to travel from one place to another in a given period of time, or to travel with a certain energy and momentum. In ...
; each vertex where lines meet gives a factor derived from an interaction term in the Lagrangian, and incoming and outgoing lines carry an energy, momentum, and
spin Spin or spinning most often refers to: * Spinning (textiles), the creation of yarn or thread by twisting fibers together, traditionally by hand spinning * Spin, the rotation of an object around a central axis * Spin (propaganda), an intentionally b ...
. In addition to their value as a mathematical tool, Feynman diagrams provide deep physical insight into the nature of particle interactions. Particles interact in every way available; in fact, intermediate virtual particles are allowed to propagate faster than light. The probability of each final state is then obtained by summing over all such possibilities. This is closely tied to the functional integral formulation of
quantum mechanics Quantum mechanics is a fundamental theory in physics that provides a description of the physical properties of nature at the scale of atoms and subatomic particles. It is the foundation of all quantum physics including quantum chemistry, qu ...
, also invented by Feynman—see
path integral formulation The path integral formulation is a description in quantum mechanics that generalizes the action principle of classical mechanics. It replaces the classical notion of a single, unique classical trajectory for a system with a sum, or functional ...
. The naïve application of such calculations often produces diagrams whose amplitudes are
infinite Infinite may refer to: Mathematics *Infinite set, a set that is not a finite set *Infinity, an abstract concept describing something without any limit Music * Infinite (group), a South Korean boy band *''Infinite'' (EP), debut EP of American m ...
, because the short-distance particle interactions require a careful limiting procedure, to include particle self-interactions. The technique of
renormalization Renormalization is a collection of techniques in quantum field theory, the statistical mechanics of fields, and the theory of self-similar geometric structures, that are used to treat infinities arising in calculated quantities by altering va ...
, suggested by
Ernst Stueckelberg Ernst Carl Gerlach Stueckelberg (baptised as Johann Melchior Ernst Karl Gerlach Stückelberg, full name after 1911: Baron Ernst Carl Gerlach Stueckelberg von Breidenbach zu Breidenstein und Melsbach; 1 February 1905 – 4 September 1984) was a S ...
and
Hans Bethe Hans Albrecht Bethe (; July 2, 1906 – March 6, 2005) was a German-American theoretical physicist who made major contributions to nuclear physics, astrophysics, quantum electrodynamics, and solid-state physics, and who won the 1967 Nobel Pr ...
and implemented by
Dyson Dyson may refer to: * Dyson (surname), people with the surname Dyson * Dyson (company), a Singaporean multinational home appliances company founded by James Dyson * Dyson (crater), a crater on the Moon * Dyson (operating system), a Unix general- ...
, Feynman, Schwinger, and Tomonaga compensates for this effect and eliminates the troublesome infinities. After renormalization, calculations using Feynman diagrams match experimental results with very high accuracy. Feynman diagram and path integral methods are also used in
statistical mechanics In physics, statistical mechanics is a mathematical framework that applies statistical methods and probability theory to large assemblies of microscopic entities. It does not assume or postulate any natural laws, but explains the macroscopic be ...
and can even be applied to
classical mechanics Classical mechanics is a physical theory describing the motion of macroscopic objects, from projectiles to parts of machinery, and astronomical objects, such as spacecraft, planets, stars, and galaxies. For objects governed by classical m ...
.


Alternative names

Murray Gell-Mann Murray Gell-Mann (; September 15, 1929 – May 24, 2019) was an American physicist who received the 1969 Nobel Prize in Physics for his work on the theory of elementary particles. He was the Robert Andrews Millikan Professor of Theoretical ...
always referred to Feynman diagrams as Stueckelberg diagrams, after a Swiss physicist,
Ernst Stueckelberg Ernst Carl Gerlach Stueckelberg (baptised as Johann Melchior Ernst Karl Gerlach Stückelberg, full name after 1911: Baron Ernst Carl Gerlach Stueckelberg von Breidenbach zu Breidenstein und Melsbach; 1 February 1905 – 4 September 1984) was a S ...
, who devised a similar notation many years earlier. Stueckelberg was motivated by the need for a manifestly covariant formalism for quantum field theory, but did not provide as automated a way to handle symmetry factors and loops, although he was first to find the correct physical interpretation in terms of forward and backward in time particle paths, all without the path-integral. Historically, as a book-keeping device of covariant perturbation theory, the graphs were called Feynman–Dyson diagrams or Dyson graphs, because the path integral was unfamiliar when they were introduced, and
Freeman Dyson Freeman John Dyson (15 December 1923 – 28 February 2020) was an English-American theoretical physicist and mathematician known for his works in quantum field theory, astrophysics, random matrices, mathematical formulation of quantum m ...
's derivation from old-fashioned perturbation theory borrowed from the perturbative expansions in statistical mechanics was easier to follow for physicists trained in earlier methods."It was Dyson's contribution to indicate how Feynman's visual insights could be used ..He realized that Feynman diagrams ..can also be viewed as a representation of the logical content of field theories (as stated in their perturbative expansions)". Schweber, op.cit (1994) Feynman had to lobby hard for the diagrams, which confused the establishment physicists trained in equations and graphs.


Representation of physical reality

In their presentations of
fundamental interactions In physics, the fundamental interactions, also known as fundamental forces, are the interactions that do not appear to be reducible to more basic interactions. There are four fundamental interactions known to exist: the gravitational and electro ...
, written from the particle physics perspective,
Gerard 't Hooft Gerardus (Gerard) 't Hooft (; born July 5, 1946) is a Dutch theoretical physicist and professor at Utrecht University, the Netherlands. He shared the 1999 Nobel Prize in Physics with his thesis advisor Martinus J. G. Veltman "for elucidating th ...
and
Martinus Veltman Martinus Justinus Godefriedus "Tini" Veltman (; 27 June 1931 – 4 January 2021) was a Dutch theoretical physicist. He shared the 1999 Nobel Prize in physics with his former PhD student Gerardus 't Hooft for their work on particle theory. Biog ...
gave good arguments for taking the original, non-regularized Feynman diagrams as the most succinct representation of our present knowledge about the physics of quantum scattering of
fundamental particles In particle physics, an elementary particle or fundamental particle is a subatomic particle that is not composed of other particles. Particles currently thought to be elementary include electrons, the fundamental fermions (quarks, leptons, anti ...
. Their motivations are consistent with the convictions of
James Daniel Bjorken James Daniel "BJ" Bjorken (born 1934) is an American theoretical physicist. He was a Putnam Fellow in 1954, received a BS in physics from MIT in 1956, and obtained his PhD from Stanford University in 1959. He was a visiting scholar at the Insti ...
and
Sidney Drell Sidney David Drell (September 13, 1926 – December 21, 2016) was an American theoretical physicist and arms control expert. At the time of his death, he was professor emeritus at the Stanford Linear Accelerator Center (SLAC) and senior fello ...
:
The Feynman graphs and rules of calculation summarize
quantum field theory In theoretical physics, quantum field theory (QFT) is a theoretical framework that combines classical field theory, special relativity, and quantum mechanics. QFT is used in particle physics to construct physical models of subatomic particles and ...
in a form in close contact with the experimental numbers one wants to understand. Although the statement of the theory in terms of graphs may imply
perturbation theory In mathematics and applied mathematics, perturbation theory comprises methods for finding an approximate solution to a problem, by starting from the exact solution of a related, simpler problem. A critical feature of the technique is a middl ...
, use of graphical methods in the
many-body problem The many-body problem is a general name for a vast category of physical problems pertaining to the properties of microscopic systems made of many interacting particles. ''Microscopic'' here implies that quantum mechanics has to be used to provi ...
shows that this formalism is flexible enough to deal with phenomena of nonperturbative characters ... Some modification of the Feynman rules of calculation may well outlive the elaborate mathematical structure of local canonical quantum field theory ...
Currently, there are no opposing opinions. In
quantum field theories In theoretical physics, quantum field theory (QFT) is a theoretical framework that combines classical field theory, special relativity, and quantum mechanics. QFT is used in particle physics to construct physical models of subatomic particles and ...
the Feynman diagrams are obtained from a Lagrangian by Feynman rules.
Dimensional regularization __NOTOC__ In theoretical physics, dimensional regularization is a method introduced by Giambiagi and Bollini as well as – independently and more comprehensively – by 't Hooft and Veltman for regularizing integrals in the evaluation of Fe ...
is a method for regularizing
integral In mathematics, an integral assigns numbers to functions in a way that describes displacement, area, volume, and other concepts that arise by combining infinitesimal data. The process of finding integrals is called integration. Along with ...
s in the evaluation of Feynman diagrams; it assigns values to them that are
meromorphic function In the mathematical field of complex analysis, a meromorphic function on an open subset ''D'' of the complex plane is a function that is holomorphic on all of ''D'' ''except'' for a set of isolated points, which are pole (complex analysis), pole ...
s of an auxiliary complex parameter , called the dimension. Dimensional regularization writes a Feynman integral as an integral depending on the spacetime dimension and spacetime points.


Particle-path interpretation

A Feynman diagram is a representation of quantum field theory processes in terms of
particle In the physical sciences, a particle (or corpuscule in older texts) is a small localized object which can be described by several physical or chemical properties, such as volume, density, or mass. They vary greatly in size or quantity, from s ...
interactions. The particles are represented by the lines of the diagram, which can be squiggly or straight, with an arrow or without, depending on the type of particle. A point where lines connect to other lines is a ''vertex'', and this is where the particles meet and interact: by emitting or absorbing new particles, deflecting one another, or changing type. There are three different types of lines: ''internal lines'' connect two vertices, ''incoming lines'' extend from "the past" to a vertex and represent an initial state, and ''outgoing lines'' extend from a vertex to "the future" and represent the final state (the latter two are also known as ''external lines''). Traditionally, the bottom of the diagram is the past and the top the future; other times, the past is to the left and the future to the right. When calculating correlation functions instead of
scattering amplitude In quantum physics, the scattering amplitude is the probability amplitude of the outgoing spherical wave relative to the incoming plane wave in a stationary-state scattering process.spacetime diagram A spacetime diagram is a graphical illustration of the properties of space and time in the special theory of relativity. Spacetime diagrams allow a qualitative understanding of the corresponding phenomena like time dilation and length contracti ...
s and bubble chamber images because they all describe particle scattering. Feynman diagrams are
graphs Graph may refer to: Mathematics *Graph (discrete mathematics), a structure made of vertices and edges **Graph theory, the study of such graphs and their properties * Graph (topology), a topological space resembling a graph in the sense of discr ...
that represent the interaction of particles rather than the physical position of the particle during a scattering process. Unlike a bubble chamber picture, only the sum of all the Feynman diagrams represent any given particle interaction; particles do not choose a particular diagram each time they interact. The law of summation is in accord with the principle of superposition—every diagram contributes to the total amplitude for the process.


Description

A Feynman diagram represents a perturbative contribution to the amplitude of a quantum transition from some initial quantum state to some final quantum state. For example, in the process of electron-positron annihilation the initial state is one electron and one positron, the final state: two photons. The initial state is often assumed to be at the left of the diagram and the final state at the right (although other conventions are also used quite often). A Feynman diagram consists of points, called vertices, and lines attached to the vertices. The particles in the initial state are depicted by lines sticking out in the direction of the initial state (e.g., to the left), the particles in the final state are represented by lines sticking out in the direction of the final state (e.g., to the right). In QED there are two types of particles: matter particles such as electrons or positrons (called
fermions In particle physics, a fermion is a particle that follows Fermi–Dirac statistics. Generally, it has a half-odd-integer spin: spin , spin , etc. In addition, these particles obey the Pauli exclusion principle. Fermions include all quarks and ...
) and exchange particles (called gauge bosons). They are represented in Feynman diagrams as follows: # Electron in the initial state is represented by a solid line, with an arrow indicating the
spin Spin or spinning most often refers to: * Spinning (textiles), the creation of yarn or thread by twisting fibers together, traditionally by hand spinning * Spin, the rotation of an object around a central axis * Spin (propaganda), an intentionally b ...
of the particle e.g. pointing toward the vertex (→•). # Electron in the final state is represented by a line, with an arrow indicating the spin of the particle e.g. pointing away from the vertex: (•→). # Positron in the initial state is represented by a solid line, with an arrow indicating the spin of the particle e.g. pointing away from the vertex: (←•). # Positron in the final state is represented by a line, with an arrow indicating the spin of the particle e.g. pointing toward the vertex: (•←). # Virtual Photon in the initial and the final state is represented by a wavy line (~• and •~). In QED a vertex always has three lines attached to it: one bosonic line, one fermionic line with arrow toward the vertex, and one fermionic line with arrow away from the vertex. The vertices might be connected by a bosonic or fermionic
propagator In quantum mechanics and quantum field theory, the propagator is a function that specifies the probability amplitude for a particle to travel from one place to another in a given period of time, or to travel with a certain energy and momentum. In ...
. A bosonic propagator is represented by a wavy line connecting two vertices (•~•). A fermionic propagator is represented by a solid line (with an arrow in one or another direction) connecting two vertices, (•←•). The number of vertices gives the order of the term in the perturbation series expansion of the transition amplitude.


Electron–positron annihilation example

The
electron–positron annihilation Electron–positron annihilation occurs when an electron () and a positron (, the electron's antiparticle) collide. At low energies, the result of the collision is the annihilation of the electron and positron, and the creation of energetic photo ...
interaction: :e+ + e → 2γ has a contribution from the second order Feynman diagram shown adjacent: In the initial state (at the bottom; early time) there is one electron (e) and one positron (e+) and in the final state (at the top; late time) there are two photons (γ).


Canonical quantization formulation

The
probability amplitude In quantum mechanics, a probability amplitude is a complex number used for describing the behaviour of systems. The modulus squared of this quantity represents a probability density. Probability amplitudes provide a relationship between the qua ...
for a transition of a quantum system (between asymptotically free states) from the initial state to the final state is given by the matrix element :S_=\langle \mathrm, S, \mathrm\rangle\;, where is the -matrix. In terms of the
time-evolution operator Time evolution is the change of state brought about by the passage of time, applicable to systems with internal state (also called ''stateful systems''). In this formulation, ''time'' is not required to be a continuous parameter, but may be disc ...
, it is simply :S=\lim _\lim _U(t_2, t_1)\;. In the
interaction picture In quantum mechanics, the interaction picture (also known as the Dirac picture after Paul Dirac) is an intermediate representation between the Schrödinger picture and the Heisenberg picture. Whereas in the other two pictures either the state ...
, this expands to :S = \mathcale^. where is the interaction Hamiltonian and signifies the time-ordered product of operators. Dyson's formula expands the time-ordered
matrix exponential In mathematics, the matrix exponential is a matrix function on square matrices analogous to the ordinary exponential function. It is used to solve systems of linear differential equations. In the theory of Lie groups, the matrix exponential gives ...
into a perturbation series in the powers of the interaction Hamiltonian density, :S=\sum_^\frac \left(\prod_^n \int d^4 x_j\right) \mathcal\left\ \equiv\sum_^S^\;. Equivalently, with the interaction Lagrangian , it is :S=\sum_^\frac \left(\prod_^n \int d^4 x_j\right) \mathcal\left\ \equiv\sum_^S^\;. A Feynman diagram is a graphical representation of a single summand in the Wick's expansion of the time-ordered product in the th-order term of the
Dyson series In scattering theory, a part of mathematical physics, the Dyson series, formulated by Freeman Dyson, is a perturbative expansion of the time evolution operator in the interaction picture. Each term can be represented by a sum of Feynman diagrams ...
of the -matrix, :\mathcal\prod_^n\mathcal_V\left(x_j\right)=\sum_(\pm)\mathcal\prod_^n\mathcal_V\left(x_j\right)\;, where signifies the normal-ordered product of the operators and (±) takes care of the possible sign change when commuting the fermionic operators to bring them together for a contraction (a
propagator In quantum mechanics and quantum field theory, the propagator is a function that specifies the probability amplitude for a particle to travel from one place to another in a given period of time, or to travel with a certain energy and momentum. In ...
) and represents all possible contractions.


Feynman rules

The diagrams are drawn according to the Feynman rules, which depend upon the interaction Lagrangian. For the QED interaction Lagrangian :L_v=-g\bar\psi\gamma^\mu\psi A_\mu describing the interaction of a fermionic field with a bosonic gauge field , the Feynman rules can be formulated in coordinate space as follows: # Each integration coordinate is represented by a point (sometimes called a vertex); # A bosonic
propagator In quantum mechanics and quantum field theory, the propagator is a function that specifies the probability amplitude for a particle to travel from one place to another in a given period of time, or to travel with a certain energy and momentum. In ...
is represented by a wiggly line connecting two points; # A fermionic propagator is represented by a solid line connecting two points; # A bosonic field A_\mu(x_i) is represented by a wiggly line attached to the point ; # A fermionic field is represented by a solid line attached to the point with an arrow toward the point; # An anti-fermionic field is represented by a solid line attached to the point with an arrow away from the point;


Example: second order processes in QED

The second order perturbation term in the -matrix is :S^=\frac\int d^4x\, d^4x'\, T\bar\psi(x)\,\gamma^\mu\,\psi(x)\,A_\mu(x)\,\bar\psi(x')\,\gamma^\nu\,\psi(x')\,A_\nu(x').\;


Scattering of fermions

The Wick's expansion of the integrand gives (among others) the following term :N\bar\psi(x)\gamma^\mu\psi(x)\bar\psi(x')\gamma^\nu\psi(x')\underline\;, where :\underline=\int\frac\frace^ is the electromagnetic contraction (propagator) in the Feynman gauge. This term is represented by the Feynman diagram at the right. This diagram gives contributions to the following processes: # e e scattering (initial state at the right, final state at the left of the diagram); # e+ e+ scattering (initial state at the left, final state at the right of the diagram); # e e+ scattering (initial state at the bottom/top, final state at the top/bottom of the diagram).


Compton scattering and annihilation/generation of e e+ pairs

Another interesting term in the expansion is :N\bar\psi(x)\,\gamma^\mu\,\underline\,\gamma^\nu\,\psi(x')\,A_\mu(x)\,A_\nu(x')\;, where :\underline=\int\frac\frace^ is the fermionic contraction (propagator).


Path integral formulation

In a path integral, the field Lagrangian, integrated over all possible field histories, defines the probability amplitude to go from one field configuration to another. In order to make sense, the field theory should have a well-defined
ground state The ground state of a quantum-mechanical system is its stationary state of lowest energy; the energy of the ground state is known as the zero-point energy of the system. An excited state is any state with energy greater than the ground state. ...
, and the integral should be performed a little bit rotated into imaginary time, i.e. a
Wick rotation In physics, Wick rotation, named after Italian physicist Gian Carlo Wick, is a method of finding a solution to a mathematical problem in Minkowski space from a solution to a related problem in Euclidean space by means of a transformation that sub ...
. The path integral formalism is completely equivalent to the canonical operator formalism above.


Scalar field Lagrangian

A simple example is the free relativistic scalar field in dimensions, whose action integral is: : S = \int \tfrac12 \partial_\mu \phi \partial^\mu \phi\, d^dx \,. The probability amplitude for a process is: : \int_A^B e^\, D\phi\,, where and are space-like hypersurfaces that define the boundary conditions. The collection of all the on the starting hypersurface give the initial value of the field, analogous to the starting position for a point particle, and the field values at each point of the final hypersurface defines the final field value, which is allowed to vary, giving a different amplitude to end up at different values. This is the field-to-field transition amplitude. The path integral gives the expectation value of operators between the initial and final state: : \int_A^B e^ \phi(x_1) \cdots \phi(x_n) \,D\phi = \left\langle A\left, \phi(x_1) \cdots \phi(x_n) \B \right\rangle\,, and in the limit that A and B recede to the infinite past and the infinite future, the only contribution that matters is from the ground state (this is only rigorously true if the path-integral is defined slightly rotated into imaginary time). The path integral can be thought of as analogous to a probability distribution, and it is convenient to define it so that multiplying by a constant doesn't change anything: : \frac = \left\langle 0 \left, \phi(x_1) \cdots \phi(x_n) \0\right\rangle \,. The normalization factor on the bottom is called the ''partition function'' for the field, and it coincides with the statistical mechanical partition function at zero temperature when rotated into imaginary time. The initial-to-final amplitudes are ill-defined if one thinks of the
continuum limit In mathematical physics and mathematics, the continuum limit or scaling limit of a lattice model refers to its behaviour in the limit as the lattice spacing goes to zero. It is often useful to use lattice models to approximate real-world processe ...
right from the beginning, because the fluctuations in the field can become unbounded. So the path-integral can be thought of as on a discrete square lattice, with lattice spacing and the limit should be taken carefully. If the final results do not depend on the shape of the lattice or the value of , then the continuum limit exists.


On a lattice

On a lattice, (i), the field can be expanded in Fourier modes: :\phi(x) = \int \frac \phi(k) e^ = \int_k \phi(k) e^\,. Here the integration domain is over restricted to a cube of side length , so that large values of are not allowed. It is important to note that the -measure contains the factors of 2 from
Fourier transform A Fourier transform (FT) is a mathematical transform that decomposes functions into frequency components, which are represented by the output of the transform as a function of frequency. Most commonly functions of time or space are transformed, ...
s, this is the best standard convention for -integrals in QFT. The lattice means that fluctuations at large are not allowed to contribute right away, they only start to contribute in the limit . Sometimes, instead of a lattice, the field modes are just cut off at high values of instead. It is also convenient from time to time to consider the space-time volume to be finite, so that the modes are also a lattice. This is not strictly as necessary as the space-lattice limit, because interactions in are not localized, but it is convenient for keeping track of the factors in front of the -integrals and the momentum-conserving delta functions that will arise. On a lattice, (ii), the action needs to be discretized: : S= \sum_ \tfrac12 \big(\phi(x) - \phi(y) \big)^2\,, where is a pair of nearest lattice neighbors and . The discretization should be thought of as defining what the derivative means. In terms of the lattice Fourier modes, the action can be written: :S= \int_k \Big( \big(1-\cos(k_1)\big) +\big(1-\cos(k_2)\big) + \cdots + \big(1-\cos(k_d)\big) \Big)\phi^*_k \phi^k\,. For near zero this is: :S = \int_k \tfrac12 k^2 \left, \phi(k)\^2\,. Now we have the continuum Fourier transform of the original action. In finite volume, the quantity is not infinitesimal, but becomes the volume of a box made by neighboring Fourier modes, or . The field is real-valued, so the Fourier transform obeys: : \phi(k)^* = \phi(-k)\,. In terms of real and imaginary parts, the real part of is an
even function In mathematics, even functions and odd functions are functions which satisfy particular symmetry relations, with respect to taking additive inverses. They are important in many areas of mathematical analysis, especially the theory of power se ...
of , while the imaginary part is odd. The Fourier transform avoids double-counting, so that it can be written: : S = \int_k \tfrac12 k^2 \phi(k) \phi(-k) over an integration domain that integrates over each pair exactly once. For a complex scalar field with action : S = \int \tfrac12 \partial_\mu\phi^* \partial^\mu\phi \,d^dx the Fourier transform is unconstrained: : S = \int_k \tfrac12 k^2 \left, \phi(k)\^2 and the integral is over all . Integrating over all different values of is equivalent to integrating over all Fourier modes, because taking a Fourier transform is a unitary linear transformation of field coordinates. When you change coordinates in a multidimensional integral by a linear transformation, the value of the new integral is given by the determinant of the transformation matrix. If : y_i = A_ x_j\,, then :\det(A) \int dx_1\, dx_2 \cdots\, dx_n = \int dy_1\, dy_2 \cdots\, dy_n\,. If is a rotation, then :A^\mathrm A = I so that , and the sign depends on whether the rotation includes a reflection or not. The matrix that changes coordinates from to can be read off from the definition of a Fourier transform. : A_ = e^ \, and the Fourier inversion theorem tells you the inverse: : A^_ = e^ \, which is the complex conjugate-transpose, up to factors of 2. On a finite volume lattice, the determinant is nonzero and independent of the field values. : \det A = 1 \, and the path integral is a separate factor at each value of . : \int \exp \left(\frac \sum_k k^2 \phi^*(k) \phi(k) \right)\, D\phi = \prod_k \int_ e^ \, The factor is the infinitesimal volume of a discrete cell in -space, in a square lattice box :d^dk = \left(\frac\right)^d\,, where is the side-length of the box. Each separate factor is an oscillatory Gaussian, and the width of the Gaussian diverges as the volume goes to infinity. In imaginary time, the ''Euclidean action'' becomes positive definite, and can be interpreted as a probability distribution. The probability of a field having values is : e^ = \prod_k e^\,. The expectation value of the field is the statistical expectation value of the field when chosen according to the probability distribution: :\left\langle \phi(x_1) \cdots \phi(x_n) \right\rangle = \frac Since the probability of is a product, the value of at each separate value of is independently Gaussian distributed. The variance of the Gaussian is , which is formally infinite, but that just means that the fluctuations are unbounded in infinite volume. In any finite volume, the integral is replaced by a discrete sum, and the variance of the integral is .


Monte Carlo

The path integral defines a probabilistic algorithm to generate a Euclidean scalar field configuration. Randomly pick the real and imaginary parts of each Fourier mode at wavenumber to be a Gaussian random variable with variance . This generates a configuration at random, and the Fourier transform gives . For real scalar fields, the algorithm must generate only one of each pair , and make the second the complex conjugate of the first. To find any correlation function, generate a field again and again by this procedure, and find the statistical average: : \left\langle \phi(x_1) \cdots \phi(x_n) \right\rangle = \lim_\frac where is the number of configurations, and the sum is of the product of the field values on each configuration. The Euclidean correlation function is just the same as the correlation function in statistics or statistical mechanics. The quantum mechanical correlation functions are an analytic continuation of the Euclidean correlation functions. For free fields with a quadratic action, the probability distribution is a high-dimensional Gaussian, and the statistical average is given by an explicit formula. But the
Monte Carlo method Monte Carlo methods, or Monte Carlo experiments, are a broad class of computational algorithms that rely on repeated random sampling to obtain numerical results. The underlying concept is to use randomness to solve problems that might be determin ...
also works well for bosonic interacting field theories where there is no closed form for the correlation functions.


Scalar propagator

Each mode is independently Gaussian distributed. The expectation of field modes is easy to calculate: : \left\langle \phi_k \phi_\right\rangle = 0 \, for , since then the two Gaussian random variables are independent and both have zero mean. : \left\langle\phi_k \phi_k \right\rangle = \frac in finite volume , when the two -values coincide, since this is the variance of the Gaussian. In the infinite volume limit, : \left\langle\phi(k) \phi(k')\right\rangle = \delta(k-k') \frac Strictly speaking, this is an approximation: the lattice propagator is: :\left\langle\phi(k) \phi(k')\right\rangle = \delta(k-k') \frac But near , for field fluctuations long compared to the lattice spacing, the two forms coincide. It is important to emphasize that the delta functions contain factors of 2, so that they cancel out the 2 factors in the measure for integrals. :\delta(k) = (2\pi)^d \delta_D(k_1)\delta_D(k_2) \cdots \delta_D(k_d) \, where is the ordinary one-dimensional Dirac delta function. This convention for delta-functions is not universal—some authors keep the factors of 2 in the delta functions (and in the -integration) explicit.


Equation of motion

The form of the propagator can be more easily found by using the equation of motion for the field. From the Lagrangian, the equation of motion is: : \partial_\mu \partial^\mu \phi = 0\, and in an expectation value, this says: :\partial_\mu\partial^\mu \left\langle \phi(x) \phi(y)\right\rangle =0 Where the derivatives act on , and the identity is true everywhere except when and coincide, and the operator order matters. The form of the singularity can be understood from the canonical commutation relations to be a delta-function. Defining the (Euclidean) ''Feynman propagator'' as the Fourier transform of the time-ordered two-point function (the one that comes from the path-integral): : \partial^2 \Delta (x) = i\delta(x)\, So that: : \Delta(k) = \frac If the equations of motion are linear, the propagator will always be the reciprocal of the quadratic-form matrix that defines the free Lagrangian, since this gives the equations of motion. This is also easy to see directly from the path integral. The factor of disappears in the Euclidean theory.


Wick theorem

Because each field mode is an independent Gaussian, the expectation values for the product of many field modes obeys ''Wick's theorem'': : \left\langle \phi(k_1) \phi(k_2) \cdots \phi(k_n)\right\rangle is zero unless the field modes coincide in pairs. This means that it is zero for an odd number of , and for an even number of , it is equal to a contribution from each pair separately, with a delta function. :\left\langle \phi(k_1) \cdots \phi(k_)\right\rangle = \sum \prod_ \frac where the sum is over each partition of the field modes into pairs, and the product is over the pairs. For example, : \left\langle \phi(k_1) \phi(k_2) \phi(k_3) \phi(k_4) \right\rangle = \frac\frac + \frac\frac + \frac\frac An interpretation of Wick's theorem is that each field insertion can be thought of as a dangling line, and the expectation value is calculated by linking up the lines in pairs, putting a delta function factor that ensures that the momentum of each partner in the pair is equal, and dividing by the propagator.


Higher Gaussian moments — completing Wick's theorem

There is a subtle point left before Wick's theorem is proved—what if more than two of the \phis have the same momentum? If it's an odd number, the integral is zero; negative values cancel with the positive values. But if the number is even, the integral is positive. The previous demonstration assumed that the \phis would only match up in pairs. But the theorem is correct even when arbitrarily many of the \phi are equal, and this is a notable property of Gaussian integration: : I = \int e^dx = \sqrt\frac : \frac I = \int \frac e^dx = \frac \sqrt\, a^ Dividing by , : \left\langle x^\right\rangle=\frac = 1 \cdot 3 \cdot 5 \ldots \cdot (2n-1) \frac : \left\langle x^2 \right\rangle = \frac If Wick's theorem were correct, the higher moments would be given by all possible pairings of a list of different : : \left\langle x_1 x_2 x_3 \cdots x_ \right\rangle where the are all the same variable, the index is just to keep track of the number of ways to pair them. The first can be paired with others, leaving . The next unpaired can be paired with different leaving , and so on. This means that Wick's theorem, uncorrected, says that the expectation value of should be: : \left\langle x^ \right\rangle = (2n-1)\cdot(2n-3)\ldots \cdot5 \cdot 3 \cdot 1 \left\langle x^2\right\rangle^n and this is in fact the correct answer. So Wick's theorem holds no matter how many of the momenta of the internal variables coincide.


Interaction

Interactions are represented by higher order contributions, since quadratic contributions are always Gaussian. The simplest interaction is the quartic self-interaction, with an action: : S = \int \partial^\mu \phi \partial_\mu\phi +\frac \phi^4. The reason for the combinatorial factor 4! will be clear soon. Writing the action in terms of the lattice (or continuum) Fourier modes: : S = \int_k k^2 \left, \phi(k)\^2 + \frac\int_ \phi(k_1) \phi(k_2) \phi(k_3)\phi(k_4) \delta(k_1+k_2+k_3 + k_4) = S_F + X. Where is the free action, whose correlation functions are given by Wick's theorem. The exponential of in the path integral can be expanded in powers of , giving a series of corrections to the free action. : e^ = e^ \left( 1 + X + \frac X X + \frac X X X + \cdots \right) The path integral for the interacting action is then a power series of corrections to the free action. The term represented by should be thought of as four half-lines, one for each factor of . The half-lines meet at a vertex, which contributes a delta-function that ensures that the sum of the momenta are all equal. To compute a correlation function in the interacting theory, there is a contribution from the terms now. For example, the path-integral for the four-field correlator: :\left\langle \phi(k_1) \phi(k_2) \phi(k_3) \phi(k_4) \right\rangle = \frac which in the free field was only nonzero when the momenta were equal in pairs, is now nonzero for all values of . The momenta of the insertions can now match up with the momenta of the s in the expansion. The insertions should also be thought of as half-lines, four in this case, which carry a momentum , but one that is not integrated. The lowest-order contribution comes from the first nontrivial term in the Taylor expansion of the action. Wick's theorem requires that the momenta in the half-lines, the factors in , should match up with the momenta of the external half-lines in pairs. The new contribution is equal to: : \lambda \frac \frac \frac \frac\,. The 4! inside is canceled because there are exactly 4! ways to match the half-lines in to the external half-lines. Each of these different ways of matching the half-lines together in pairs contributes exactly once, regardless of the values of , by Wick's theorem.


Feynman diagrams

The expansion of the action in powers of gives a series of terms with progressively higher number of s. The contribution from the term with exactly s is called th order. The th order terms has: # internal half-lines, which are the factors of from the s. These all end on a vertex, and are integrated over all possible . # external half-lines, which are the come from the insertions in the integral. By Wick's theorem, each pair of half-lines must be paired together to make a ''line'', and this line gives a factor of : \frac which multiplies the contribution. This means that the two half-lines that make a line are forced to have equal and opposite momentum. The line itself should be labelled by an arrow, drawn parallel to the line, and labeled by the momentum in the line . The half-line at the tail end of the arrow carries momentum , while the half-line at the head-end carries momentum . If one of the two half-lines is external, this kills the integral over the internal , since it forces the internal to be equal to the external . If both are internal, the integral over remains. The diagrams that are formed by linking the half-lines in the s with the external half-lines, representing insertions, are the Feynman diagrams of this theory. Each line carries a factor of , the propagator, and either goes from vertex to vertex, or ends at an insertion. If it is internal, it is integrated over. At each vertex, the total incoming is equal to the total outgoing . The number of ways of making a diagram by joining half-lines into lines almost completely cancels the factorial factors coming from the Taylor series of the exponential and the 4! at each vertex.


Loop order

A forest diagram is one where all the internal lines have momentum that is completely determined by the external lines and the condition that the incoming and outgoing momentum are equal at each vertex. The contribution of these diagrams is a product of propagators, without any integration. A tree diagram is a connected forest diagram. An example of a tree diagram is the one where each of four external lines end on an . Another is when three external lines end on an , and the remaining half-line joins up with another , and the remaining half-lines of this run off to external lines. These are all also forest diagrams (as every tree is a forest); an example of a forest that is not a tree is when eight external lines end on two s. It is easy to verify that in all these cases, the momenta on all the internal lines is determined by the external momenta and the condition of momentum conservation in each vertex. A diagram that is not a forest diagram is called a ''loop'' diagram, and an example is one where two lines of an are joined to external lines, while the remaining two lines are joined to each other. The two lines joined to each other can have any momentum at all, since they both enter and leave the same vertex. A more complicated example is one where two s are joined to each other by matching the legs one to the other. This diagram has no external lines at all. The reason loop diagrams are called loop diagrams is because the number of -integrals that are left undetermined by momentum conservation is equal to the number of independent closed loops in the diagram, where independent loops are counted as in
homology theory In mathematics, homology is a general way of associating a sequence of algebraic objects, such as abelian groups or modules, with other mathematical objects such as topological spaces. Homology groups were originally defined in algebraic topol ...
. The homology is real-valued (actually valued), the value associated with each line is the momentum. The boundary operator takes each line to the sum of the end-vertices with a positive sign at the head and a negative sign at the tail. The condition that the momentum is conserved is exactly the condition that the boundary of the -valued weighted graph is zero. A set of valid -values can be arbitrarily redefined whenever there is a closed loop. A closed loop is a cyclical path of adjacent vertices that never revisits the same vertex. Such a cycle can be thought of as the boundary of a hypothetical 2-cell. The -labellings of a graph that conserve momentum (i.e. which has zero boundary) up to redefinitions of (i.e. up to boundaries of 2-cells) define the first homology of a graph. The number of independent momenta that are not determined is then equal to the number of independent homology loops. For many graphs, this is equal to the number of loops as counted in the most intuitive way.


Symmetry factors

The number of ways to form a given Feynman diagram by joining together half-lines is large, and by Wick's theorem, each way of pairing up the half-lines contributes equally. Often, this completely cancels the factorials in the denominator of each term, but the cancellation is sometimes incomplete. The uncancelled denominator is called the ''symmetry factor'' of the diagram. The contribution of each diagram to the correlation function must be divided by its symmetry factor. For example, consider the Feynman diagram formed from two external lines joined to one , and the remaining two half-lines in the joined to each other. There are 4 × 3 ways to join the external half-lines to the , and then there is only one way to join the two remaining lines to each other. The comes divided by , but the number of ways to link up the half lines to make the diagram is only 4 × 3, so the contribution of this diagram is divided by two. For another example, consider the diagram formed by joining all the half-lines of one to all the half-lines of another . This diagram is called a ''vacuum bubble'', because it does not link up to any external lines. There are 4! ways to form this diagram, but the denominator includes a 2! (from the expansion of the exponential, there are two s) and two factors of 4!. The contribution is multiplied by = . Another example is the Feynman diagram formed from two s where each links up to two external lines, and the remaining two half-lines of each are joined to each other. The number of ways to link an to two external lines is 4 × 3, and either could link up to either pair, giving an additional factor of 2. The remaining two half-lines in the two s can be linked to each other in two ways, so that the total number of ways to form the diagram is , while the denominator is . The total symmetry factor is 2, and the contribution of this diagram is divided by 2. The symmetry factor theorem gives the symmetry factor for a general diagram: the contribution of each Feynman diagram must be divided by the order of its group of automorphisms, the number of symmetries that it has. An
automorphism In mathematics, an automorphism is an isomorphism from a mathematical object to itself. It is, in some sense, a symmetry of the object, and a way of mapping the object to itself while preserving all of its structure. The set of all automorphis ...
of a Feynman graph is a permutation of the lines and a permutation of the vertices with the following properties: # If a line goes from vertex to vertex , then goes from to . If the line is undirected, as it is for a real scalar field, then can go from to too. # If a line ends on an external line, ends on the same external line. # If there are different types of lines, should preserve the type. This theorem has an interpretation in terms of particle-paths: when identical particles are present, the integral over all intermediate particles must not double-count states that differ only by interchanging identical particles. Proof: To prove this theorem, label all the internal and external lines of a diagram with a unique name. Then form the diagram by linking a half-line to a name and then to the other half line. Now count the number of ways to form the named diagram. Each permutation of the s gives a different pattern of linking names to half-lines, and this is a factor of . Each permutation of the half-lines in a single gives a factor of 4!. So a named diagram can be formed in exactly as many ways as the denominator of the Feynman expansion. But the number of unnamed diagrams is smaller than the number of named diagram by the order of the automorphism group of the graph.


Connected diagrams: ''linked-cluster theorem''

Roughly speaking, a Feynman diagram is called ''connected'' if all vertices and propagator lines are linked by a sequence of vertices and propagators of the diagram itself. If one views it as an
undirected graph In discrete mathematics, and more specifically in graph theory, a graph is a structure amounting to a set of objects in which some pairs of the objects are in some sense "related". The objects correspond to mathematical abstractions called '' v ...
it is connected. The remarkable relevance of such diagrams in QFTs is due to the fact that they are sufficient to determine the quantum partition function . More precisely, connected Feynman diagrams determine :i W equiv \ln Z To see this, one should recall that : Z propto\sum_k with constructed from some (arbitrary) Feynman diagram that can be thought to consist of several connected components . If one encounters (identical) copies of a component within the Feynman diagram one has to include a ''symmetry factor'' . However, in the end each contribution of a Feynman diagram to the partition function has the generic form :\prod_i \frac where labels the (infinitely) many connected Feynman diagrams possible. A scheme to successively create such contributions from the to is obtained by :\left(\frac+\frac+\frac+\cdots\right)\left(1+C_2+\fracC^2_2+\cdots\right)\cdots and therefore yields :Z propto\prod_i=\exp\propto \exp\,. To establish the ''normalization'' one simply calculates all connected ''vacuum diagrams'', i.e., the diagrams without any ''sources'' (sometimes referred to as ''external legs'' of a Feynman diagram).


Vacuum bubbles

An immediate consequence of the linked-cluster theorem is that all vacuum bubbles, diagrams without external lines, cancel when calculating correlation functions. A correlation function is given by a ratio of path-integrals: : \left\langle \phi_1(x_1) \cdots \phi_n(x_n)\right\rangle = \frac\,. The top is the sum over all Feynman diagrams, including disconnected diagrams that do not link up to external lines at all. In terms of the connected diagrams, the numerator includes the same contributions of vacuum bubbles as the denominator: : \int e^\phi_1(x_1)\cdots\phi_n(x_n)\, D\phi = \left(\sum E_i\right)\left( \exp\left(\sum_i C_i\right) \right)\,. Where the sum over diagrams includes only those diagrams each of whose connected components end on at least one external line. The vacuum bubbles are the same whatever the external lines, and give an overall multiplicative factor. The denominator is the sum over all vacuum bubbles, and dividing gets rid of the second factor. The vacuum bubbles then are only useful for determining itself, which from the definition of the path integral is equal to: : Z= \int e^ D\phi = e^ = e^ where is the energy density in the vacuum. Each vacuum bubble contains a factor of zeroing the total at each vertex, and when there are no external lines, this contains a factor of , because the momentum conservation is over-enforced. In finite volume, this factor can be identified as the total volume of space time. Dividing by the volume, the remaining integral for the vacuum bubble has an interpretation: it is a contribution to the energy density of the vacuum.


Sources

Correlation functions are the sum of the connected Feynman diagrams, but the formalism treats the connected and disconnected diagrams differently. Internal lines end on vertices, while external lines go off to insertions. Introducing ''sources'' unifies the formalism, by making new vertices where one line can end. Sources are external fields, fields that contribute to the action, but are not dynamical variables. A scalar field source is another scalar field that contributes a term to the (Lorentz) Lagrangian: : \int h(x) \phi(x)\, d^dx = \int h(k) \phi(k)\, d^dk \, In the Feynman expansion, this contributes H terms with one half-line ending on a vertex. Lines in a Feynman diagram can now end either on an vertex, or on an vertex, and only one line enters an vertex. The Feynman rule for an vertex is that a line from an with momentum gets a factor of . The sum of the connected diagrams in the presence of sources includes a term for each connected diagram in the absence of sources, except now the diagrams can end on the source. Traditionally, a source is represented by a little "×" with one line extending out, exactly as an insertion. : \log\big(Z big) = \sum_ h(k_1) h(k_2) \cdots h(k_n) C(k_1,\cdots,k_n)\, where is the connected diagram with external lines carrying momentum as indicated. The sum is over all connected diagrams, as before. The field is not dynamical, which means that there is no path integral over : is just a parameter in the Lagrangian, which varies from point to point. The path integral for the field is: : Z = \int e^\, D\phi \, and it is a function of the values of at every point. One way to interpret this expression is that it is taking the Fourier transform in field space. If there is a probability density on , the Fourier transform of the probability density is: : \int \rho(y) e^\, d^n y = \left\langle e^ \right\rangle = \left\langle \prod_^ e^\right\rangle \, The Fourier transform is the expectation of an oscillatory exponential. The path integral in the presence of a source is: : Z = \int e^ e^\, D\phi = \left\langle e^\right\rangle which, on a lattice, is the product of an oscillatory exponential for each field value: : \left\langle \prod_x e^\right\rangle The Fourier transform of a delta-function is a constant, which gives a formal expression for a delta function: : \delta(x-y) = \int e^\, dk This tells you what a field delta function looks like in a path-integral. For two scalar fields and , : \delta(\phi - \eta) = \int e^\, Dh\,, which integrates over the Fourier transform coordinate, over . This expression is useful for formally changing field coordinates in the path integral, much as a delta function is used to change coordinates in an ordinary multi-dimensional integral. The partition function is now a function of the field , and the physical partition function is the value when is the zero function: The correlation functions are derivatives of the path integral with respect to the source: : \left\langle\phi(x)\right\rangle = \frac \frac Z = \frac \log\big(Z big)\,. In Euclidean space, source contributions to the action can still appear with a factor of , so that they still do a Fourier transform.


Spin ; "photons" and "ghosts"


Spin : Grassmann integrals

The field path integral can be extended to the Fermi case, but only if the notion of integration is expanded. A Grassmann integral of a free Fermi field is a high-dimensional
determinant In mathematics, the determinant is a scalar value that is a function of the entries of a square matrix. It characterizes some properties of the matrix and the linear map represented by the matrix. In particular, the determinant is nonzero if an ...
or
Pfaffian In mathematics, the determinant of a skew-symmetric matrix can always be written as the square of a polynomial in the matrix entries, a polynomial with integer coefficients that only depend on the size of the matrix. The value of this polynomial, ...
, which defines the new type of Gaussian integration appropriate for Fermi fields. The two fundamental formulas of Grassmann integration are: : \int e^\, D\bar\psi\, D\psi= \mathrm(M)\,, where is an arbitrary matrix and are independent Grassmann variables for each index , and : \int e^\, D\psi = \mathrm(A)\,, where is an antisymmetric matrix, is a collection of Grassmann variables, and the is to prevent double-counting (since ). In matrix notation, where and are Grassmann-valued row vectors, and are Grassmann-valued column vectors, and is a real-valued matrix: : Z = \int e^\, D\bar\psi\, D\psi = \int e^\, D\bar\psi\, D\psi = \mathrm(M) e^\,, where the last equality is a consequence of the translation invariance of the Grassmann integral. The Grassmann variables are external sources for , and differentiating with respect to pulls down factors of . : \left\langle\bar\psi \psi\right\rangle = \frac \frac \frac Z , _ = M^ again, in a schematic matrix notation. The meaning of the formula above is that the derivative with respect to the appropriate component of and gives the matrix element of . This is exactly analogous to the bosonic path integration formula for a Gaussian integral of a complex bosonic field: : \int e^ \,D\phi^*\, D\phi = \frac : \left\langle\phi^* \phi\right\rangle = \frac \frac \fracZ , _ = M^ \,. So that the propagator is the inverse of the matrix in the quadratic part of the action in both the Bose and Fermi case. For real Grassmann fields, for
Majorana fermion A Majorana fermion (, uploaded 19 April 2013, retrieved 5 October 2014; and also based on the pronunciation of physicist's name.), also referred to as a Majorana particle, is a fermion that is its own antiparticle. They were hypothesised by Et ...
s, the path integral is a Pfaffian times a source quadratic form, and the formulas give the square root of the determinant, just as they do for real Bosonic fields. The propagator is still the inverse of the quadratic part. The free Dirac Lagrangian: : \int \bar\psi\left(\gamma^\mu \partial_ - m \right) \psi formally gives the equations of motion and the anticommutation relations of the Dirac field, just as the Klein Gordon Lagrangian in an ordinary path integral gives the equations of motion and commutation relations of the scalar field. By using the spatial Fourier transform of the Dirac field as a new basis for the Grassmann algebra, the quadratic part of the Dirac action becomes simple to invert: : S= \int_k \bar\psi\left( i\gamma^\mu k_\mu - m \right) \psi\,. The propagator is the inverse of the matrix linking and , since different values of do not mix together. : \left\langle\bar\psi(k') \psi (k) \right\rangle = \delta (k+k')\frac = \delta(k+k')\frac The analog of Wick's theorem matches and in pairs: : \left\langle\bar\psi(k_1) \bar\psi(k_2) \cdots \bar\psi(k_n) \psi(k'_1) \cdots \psi(k_n)\right\rangle = \sum_ (-1)^S \prod_ \delta\left(k_i -k_j\right) \frac where S is the sign of the permutation that reorders the sequence of and to put the ones that are paired up to make the delta-functions next to each other, with the coming right before the . Since a pair is a commuting element of the Grassmann algebra, it doesn't matter what order the pairs are in. If more than one pair have the same , the integral is zero, and it is easy to check that the sum over pairings gives zero in this case (there are always an even number of them). This is the Grassmann analog of the higher Gaussian moments that completed the Bosonic Wick's theorem earlier. The rules for spin- Dirac particles are as follows: The propagator is the inverse of the Dirac operator, the lines have arrows just as for a complex scalar field, and the diagram acquires an overall factor of −1 for each closed Fermi loop. If there are an odd number of Fermi loops, the diagram changes sign. Historically, the −1 rule was very difficult for Feynman to discover. He discovered it after a long process of trial and error, since he lacked a proper theory of Grassmann integration. The rule follows from the observation that the number of Fermi lines at a vertex is always even. Each term in the Lagrangian must always be Bosonic. A Fermi loop is counted by following Fermionic lines until one comes back to the starting point, then removing those lines from the diagram. Repeating this process eventually erases all the Fermionic lines: this is the Euler algorithm to 2-color a graph, which works whenever each vertex has even degree. The number of steps in the Euler algorithm is only equal to the number of independent Fermionic homology cycles in the common special case that all terms in the Lagrangian are exactly quadratic in the Fermi fields, so that each vertex has exactly two Fermionic lines. When there are four-Fermi interactions (like in the Fermi effective theory of the weak nuclear interactions) there are more -integrals than Fermi loops. In this case, the counting rule should apply the Euler algorithm by pairing up the Fermi lines at each vertex into pairs that together form a bosonic factor of the term in the Lagrangian, and when entering a vertex by one line, the algorithm should always leave with the partner line. To clarify and prove the rule, consider a Feynman diagram formed from vertices, terms in the Lagrangian, with Fermion fields. The full term is Bosonic, it is a commuting element of the Grassmann algebra, so the order in which the vertices appear is not important. The Fermi lines are linked into loops, and when traversing the loop, one can reorder the vertex terms one after the other as one goes around without any sign cost. The exception is when you return to the starting point, and the final half-line must be joined with the unlinked first half-line. This requires one permutation to move the last to go in front of the first , and this gives the sign. This rule is the only visible effect of the exclusion principle in internal lines. When there are external lines, the amplitudes are antisymmetric when two Fermi insertions for identical particles are interchanged. This is automatic in the source formalism, because the sources for Fermi fields are themselves Grassmann valued.


Spin 1: photons

The naive propagator for photons is infinite, since the Lagrangian for the A-field is: : S = \int \tfrac14 F^ F_ = \int -\tfrac12\left(\partial^\mu A_\nu \partial_\mu A^\nu - \partial^\mu A_\mu \partial_\nu A^\nu \right)\,. The quadratic form defining the propagator is non-invertible. The reason is the
gauge invariance In physics, a gauge theory is a type of field theory in which the Lagrangian (and hence the dynamics of the system itself) does not change (is invariant) under local transformations according to certain smooth families of operations (Lie grou ...
of the field; adding a gradient to does not change the physics. To fix this problem, one needs to fix a gauge. The most convenient way is to demand that the divergence of is some function , whose value is random from point to point. It does no harm to integrate over the values of , since it only determines the choice of gauge. This procedure inserts the following factor into the path integral for : : \int \delta\left(\partial_\mu A^\mu - f\right) e^\, Df\,. The first factor, the delta function, fixes the gauge. The second factor sums over different values of that are inequivalent gauge fixings. This is simply : e^\,. The additional contribution from gauge-fixing cancels the second half of the free Lagrangian, giving the Feynman Lagrangian: : S= \int \partial^\mu A^\nu \partial_\mu A_\nu which is just like four independent free scalar fields, one for each component of . The Feynman propagator is: : \left\langle A_\mu(k) A_\nu(k') \right\rangle = \delta\left(k+k'\right) \frac. The one difference is that the sign of one propagator is wrong in the Lorentz case: the timelike component has an opposite sign propagator. This means that these particle states have negative norm—they are not physical states. In the case of photons, it is easy to show by diagram methods that these states are not physical—their contribution cancels with longitudinal photons to only leave two physical photon polarization contributions for any value of . If the averaging over is done with a coefficient different from , the two terms don't cancel completely. This gives a covariant Lagrangian with a coefficient \lambda, which does not affect anything: : S= \int \tfrac12\left(\partial^\mu A^\nu \partial_\mu A_\nu - \lambda \left(\partial_\mu A^\mu\right)^2\right) and the covariant propagator for QED is: :\left \langle A_\mu(k) A_\nu(k') \right\rangle =\delta\left(k+k'\right)\frac.


Spin 1: non-Abelian ghosts

To find the Feynman rules for non-Abelian gauge fields, the procedure that performs the gauge fixing must be carefully corrected to account for a change of variables in the path-integral. The gauge fixing factor has an extra determinant from popping the delta function: : \delta\left(\partial_\mu A_\mu - f\right) e^ \det M To find the form of the determinant, consider first a simple two-dimensional integral of a function that depends only on , not on the angle . Inserting an integral over : : \int f(r)\, dx\, dy = \int f(r) \int d\theta\, \delta(y) \left, \frac\\, dx\, dy The derivative-factor ensures that popping the delta function in removes the integral. Exchanging the order of integration, : \int f(r)\, dx\, dy = \int d\theta\, \int f(r) \delta(y) \left, \frac\\, dx\, dy but now the delta-function can be popped in , : \int f(r)\, dx\, dy = \int d\theta_0\, \int f(x) \left, \frac\\, dx\,. The integral over just gives an overall factor of 2, while the rate of change of with a change in is just , so this exercise reproduces the standard formula for polar integration of a radial function: : \int f(r)\, dx\, dy = 2\pi \int f(x) x\, dx In the path-integral for a nonabelian gauge field, the analogous manipulation is: : \int DA \int \delta\big(F(A)\big) \det\left(\frac\right)\, DG e^ = \int DG \int \delta\big(F(A)\big)\det\left(\frac\right) e^ \, The factor in front is the volume of the gauge group, and it contributes a constant, which can be discarded. The remaining integral is over the gauge fixed action. : \int \det\left(\frac\right)e^\, DA \, To get a covariant gauge, the gauge fixing condition is the same as in the Abelian case: : \partial_\mu A^\mu = f \,, Whose variation under an infinitesimal gauge transformation is given by: : \partial_\mu\, D_\mu \alpha \,, where is the adjoint valued element of the Lie algebra at every point that performs the infinitesimal gauge transformation. This adds the Faddeev Popov determinant to the action: : \det\left(\partial_\mu\, D_\mu\right) \, which can be rewritten as a Grassmann integral by introducing ghost fields: : \int e^\, D\bar\eta\, D\eta \, The determinant is independent of , so the path-integral over can give the Feynman propagator (or a covariant propagator) by choosing the measure for as in the abelian case. The full gauge fixed action is then the Yang Mills action in Feynman gauge with an additional ghost action: : S= \int \operatorname \partial_\mu A_\nu \partial^\mu A^\nu + f^i_ \partial^\nu A_i^\mu A^j_\mu A^k_\nu + f^i_ f^r_ A_i A_j A^k A^l + \operatorname \partial_\mu \bar\eta \partial^\mu \eta + \bar\eta A_j \eta \, The diagrams are derived from this action. The propagator for the spin-1 fields has the usual Feynman form. There are vertices of degree 3 with momentum factors whose couplings are the structure constants, and vertices of degree 4 whose couplings are products of structure constants. There are additional ghost loops, which cancel out timelike and longitudinal states in loops. In the Abelian case, the determinant for covariant gauges does not depend on , so the ghosts do not contribute to the connected diagrams.


Particle-path representation

Feynman diagrams were originally discovered by Feynman, by trial and error, as a way to represent the contribution to the S-matrix from different classes of particle trajectories.


Schwinger representation

The Euclidean scalar propagator has a suggestive representation: : \frac = \int_0^\infty e^\, d\tau The meaning of this identity (which is an elementary integration) is made clearer by Fourier transforming to real space. : \Delta(x) = \int_0^\infty d\tau e^ \frace^\frac The contribution at any one value of to the propagator is a Gaussian of width . The total propagation function from 0 to is a weighted sum over all proper times of a normalized Gaussian, the probability of ending up at after a random walk of time . The path-integral representation for the propagator is then: : \Delta(x) = \int_0^\infty d\tau \int DX\, e^ which is a path-integral rewrite of the Schwinger representation. The Schwinger representation is both useful for making manifest the particle aspect of the propagator, and for symmetrizing denominators of loop diagrams.


Combining denominators

The Schwinger representation has an immediate practical application to loop diagrams. For example, for the diagram in the theory formed by joining two s together in two half-lines, and making the remaining lines external, the integral over the internal propagators in the loop is: : \int_k \frac \frac \,. Here one line carries momentum and the other . The asymmetry can be fixed by putting everything in the Schwinger representation. : \int_ e^\, dt\, dt'\,. Now the exponent mostly depends on , : \int_ e^\,, except for the asymmetrical little bit. Defining the variable and , the variable goes from 0 to , while goes from 0 to 1. The variable is the total proper time for the loop, while parametrizes the fraction of the proper time on the top of the loop versus the bottom. The Jacobian for this transformation of variables is easy to work out from the identities: : d(uv)= dt'\quad du = dt+dt'\,, and " wedging" gives : u\, du \wedge dv = dt \wedge dt'\,. This allows the integral to be evaluated explicitly: : \int_ u e^ = \int \frac\, dv leaving only the -integral. This method, invented by Schwinger but usually attributed to Feynman, is called ''combining denominator''. Abstractly, it is the elementary identity: : \frac= \int_0^1 \frac\, dv But this form does not provide the physical motivation for introducing ; is the proportion of proper time on one of the legs of the loop. Once the denominators are combined, a shift in to symmetrizes everything: : \int_0^1 \int\frac\, dk\, dv = \int_0^1 \int \frac\, dk'\, dv This form shows that the moment that is more negative than four times the mass of the particle in the loop, which happens in a physical region of
Lorentz space In mathematical analysis, Lorentz spaces, introduced by George G. Lorentz in the 1950s,G. Lorentz, "On the theory of spaces Λ", ''Pacific Journal of Mathematics'' 1 (1951), pp. 411-429. are generalisations of the more familiar L^ spaces. The Lor ...
, the integral has a cut. This is exactly when the external momentum can create physical particles. When the loop has more vertices, there are more denominators to combine: : \int dk\, \frac \frac \cdots \frac The general rule follows from the Schwinger prescription for denominators: : \frac = \int_0^\infty \cdots\int_0^\infty e^\, du_0 \cdots du_n \,. The integral over the Schwinger parameters can be split up as before into an integral over the total proper time and an integral over the fraction of the proper time in all but the first segment of the loop for . The are positive and add up to less than 1, so that the integral is over an -dimensional simplex. The Jacobian for the coordinate transformation can be worked out as before: : du = du_0 + du_1 \cdots + du_n \, : d(uv_i) = d u_i \,. Wedging all these equations together, one obtains : u^n\, du \wedge dv_1 \wedge dv_2 \cdots \wedge dv_n = du_0 \wedge du_1 \cdots \wedge du_n \,. This gives the integral: : \int_0^\infty \int_ u^n e^\, dv_1\cdots dv_n\, du\,, where the simplex is the region defined by the conditions :v_i>0 \quad \mbox \quad \sum_^n v_i < 1 as well as :v_0 = 1-\sum_^n v_i\,. Performing the integral gives the general prescription for combining denominators: : \frac = n! \int_ \frac\, dv_1\, dv_2 \cdots dv_n Since the numerator of the integrand is not involved, the same prescription works for any loop, no matter what the spins are carried by the legs. The interpretation of the parameters is that they are the fraction of the total proper time spent on each leg.


Scattering

The correlation functions of a quantum field theory describe the scattering of particles. The definition of "particle" in relativistic field theory is not self-evident, because if you try to determine the position so that the uncertainty is less than the
compton wavelength The Compton wavelength is a quantum mechanical property of a particle. The Compton wavelength of a particle is equal to the wavelength of a photon whose energy is the same as the rest energy of that particle (see mass–energy equivalence). It wa ...
, the uncertainty in energy is large enough to produce more particles and antiparticles of the same type from the vacuum. This means that the notion of a single-particle state is to some extent incompatible with the notion of an object localized in space. In the 1930s,
Wigner Eugene Paul "E. P." Wigner ( hu, Wigner Jenő Pál, ; November 17, 1902 – January 1, 1995) was a Hungarian-American theoretical physicist who also contributed to mathematical physics. He received the Nobel Prize in Physics in 1963 "for his con ...
gave a mathematical definition for single-particle states: they are a collection of states that form an irreducible representation of the Poincaré group. Single particle states describe an object with a finite mass, a well defined momentum, and a spin. This definition is fine for protons and neutrons, electrons and photons, but it excludes quarks, which are permanently confined, so the modern point of view is more accommodating: a particle is anything whose interaction can be described in terms of Feynman diagrams, which have an interpretation as a sum over particle trajectories. A field operator can act to produce a one-particle state from the vacuum, which means that the field operator produces a superposition of Wigner particle states. In the free field theory, the field produces one particle states only. But when there are interactions, the field operator can also produce 3-particle, 5-particle (if there is no +/− symmetry also 2, 4, 6 particle) states too. To compute the scattering amplitude for single particle states only requires a careful limit, sending the fields to infinity and integrating over space to get rid of the higher-order corrections. The relation between scattering and correlation functions is the LSZ-theorem: The scattering amplitude for particles to go to particles in a scattering event is the given by the sum of the Feynman diagrams that go into the correlation function for field insertions, leaving out the propagators for the external legs. For example, for the interaction of the previous section, the order contribution to the (Lorentz) correlation function is: : \left\langle \phi(k_1)\phi(k_2)\phi(k_3)\phi(k_4)\right\rangle = \frac\frac \frac \frac i\lambda \, Stripping off the external propagators, that is, removing the factors of , gives the invariant scattering amplitude : : M = i\lambda \, which is a constant, independent of the incoming and outgoing momentum. The interpretation of the scattering amplitude is that the sum of over all possible final states is the probability for the scattering event. The normalization of the single-particle states must be chosen carefully, however, to ensure that is a relativistic invariant. Non-relativistic single particle states are labeled by the momentum , and they are chosen to have the same norm at every value of . This is because the nonrelativistic unit operator on single particle states is: : \int dk\, , k\rangle\langle k, \,. In relativity, the integral over the -states for a particle of mass m integrates over a hyperbola in space defined by the energy–momentum relation: : E^2 - k^2 = m^2 \,. If the integral weighs each point equally, the measure is not Lorentz-invariant. The invariant measure integrates over all values of and , restricting to the hyperbola with a Lorentz-invariant delta function: : \int \delta(E^2-k^2 - m^2) , E,k\rangle\langle E,k, \, dE\, dk = \int , k\rangle\langle k, \,. So the normalized -states are different from the relativistically normalized -states by a factor of :\sqrt = \left(k^2-m^2\right)^\frac14\,. The invariant amplitude is then the probability amplitude for relativistically normalized incoming states to become relativistically normalized outgoing states. For nonrelativistic values of , the relativistic normalization is the same as the nonrelativistic normalization (up to a constant factor ). In this limit, the invariant scattering amplitude is still constant. The particles created by the field scatter in all directions with equal amplitude. The nonrelativistic potential, which scatters in all directions with an equal amplitude (in the Born approximation), is one whose Fourier transform is constant—a delta-function potential. The lowest order scattering of the theory reveals the non-relativistic interpretation of this theory—it describes a collection of particles with a delta-function repulsion. Two such particles have an aversion to occupying the same point at the same time.


Nonperturbative effects

Thinking of Feynman diagrams as a perturbation series, nonperturbative effects like tunneling do not show up, because any effect that goes to zero faster than any polynomial does not affect the Taylor series. Even bound states are absent, since at any finite order particles are only exchanged a finite number of times, and to make a bound state, the binding force must last forever. But this point of view is misleading, because the diagrams not only describe scattering, but they also are a representation of the short-distance field theory correlations. They encode not only asymptotic processes like particle scattering, they also describe the multiplication rules for fields, the
operator product expansion In quantum field theory, the operator product expansion (OPE) is used as an axiom to define the product of fields as a sum over the same fields. As an axiom, it offers a non-perturbative approach to quantum field theory. One example is the vert ...
. Nonperturbative tunneling processes involve field configurations that on average get big when the
coupling constant In physics, a coupling constant or gauge coupling parameter (or, more simply, a coupling), is a number that determines the strength of the force exerted in an interaction. Originally, the coupling constant related the force acting between two ...
gets small, but each configuration is a
coherent Coherence, coherency, or coherent may refer to the following: Physics * Coherence (physics), an ideal property of waves that enables stationary (i.e. temporally and spatially constant) interference * Coherence (units of measurement), a deriv ...
superposition of particles whose local interactions are described by Feynman diagrams. When the coupling is small, these become collective processes that involve large numbers of particles, but where the interactions between each of the particles is simple. (The perturbation series of any interacting quantum field theory has zero
radius of convergence In mathematics, the radius of convergence of a power series is the radius of the largest disk at the center of the series in which the series converges. It is either a non-negative real number or \infty. When it is positive, the power series ...
, complicating the limit of the infinite series of diagrams needed (in the limit of vanishing coupling) to describe such field configurations.) This means that nonperturbative effects show up asymptotically in resummations of infinite classes of diagrams, and these diagrams can be locally simple. The graphs determine the local equations of motion, while the allowed large-scale configurations describe non-perturbative physics. But because Feynman propagators are nonlocal in time, translating a field process to a coherent particle language is not completely intuitive, and has only been explicitly worked out in certain special cases. In the case of nonrelativistic
bound state Bound or bounds may refer to: Mathematics * Bound variable * Upper and lower bounds, observed limits of mathematical functions Physics * Bound state, a particle that has a tendency to remain localized in one or more regions of space Geography * ...
s, the Bethe–Salpeter equation describes the class of diagrams to include to describe a relativistic atom. For
quantum chromodynamics In theoretical physics, quantum chromodynamics (QCD) is the theory of the strong interaction between quarks mediated by gluons. Quarks are fundamental particles that make up composite hadrons such as the proton, neutron and pion. QCD is a type o ...
, the Shifman–Vainshtein–Zakharov sum rules describe non-perturbatively excited long-wavelength field modes in particle language, but only in a phenomenological way. The number of Feynman diagrams at high orders of perturbation theory is very large, because there are as many diagrams as there are graphs with a given number of nodes. Nonperturbative effects leave a signature on the way in which the number of diagrams and resummations diverge at high order. It is only because non-perturbative effects appear in hidden form in diagrams that it was possible to analyze nonperturbative effects in string theory, where in many cases a Feynman description is the only one available.


In popular culture

* The use of the above diagram of the virtual particle producing a
quark A quark () is a type of elementary particle and a fundamental constituent of matter. Quarks combine to form composite particles called hadrons, the most stable of which are protons and neutrons, the components of atomic nuclei. All commonly o ...
antiquark A quark () is a type of elementary particle and a fundamental constituent of matter. Quarks combine to form composite particles called hadrons, the most stable of which are protons and neutrons, the components of atomic nuclei. All commonly ...
pair was featured in the television sit-com ''
The Big Bang Theory ''The Big Bang Theory'' is an American television sitcom created by Chuck Lorre and Bill Prady, both of whom served as executive producers on the series, along with Steven Molaro, all of whom also served as head writers. It premiered on CBS ...
'', in the episode "The Bat Jar Conjecture". * '' PhD Comics'' of January 11, 2012, shows Feynman diagrams that ''visualize and describe quantum academic interactions'', i.e. the paths followed by Ph.D. students when interacting with their advisors. * '' Vacuum Diagrams'' a science fiction story by Stephen Baxter features the titular vacuum diagram, a specific type of Feynman diagram. * Feynman and his wife, Gweneth Howarth, bought a Dodge Tradesman Maxivan in 1975, and had it painted with Feynman diagrams.


See also

* One-loop Feynman diagram * Julian Schwinger#Schwinger and Feynman * Stueckelberg–Feynman interpretation *
Penguin diagram In quantum field theory, penguin diagrams are a class of Feynman diagrams which are important for understanding CP violating processes in the standard model. They refer to one-loop processes in which a quark temporarily changes flavor (via a W ...
*
Path integral formulation The path integral formulation is a description in quantum mechanics that generalizes the action principle of classical mechanics. It replaces the classical notion of a single, unique classical trajectory for a system with a sum, or functional ...
*
Propagator In quantum mechanics and quantum field theory, the propagator is a function that specifies the probability amplitude for a particle to travel from one place to another in a given period of time, or to travel with a certain energy and momentum. In ...
*
List of Feynman diagrams This is a list of common Feynman diagram In theoretical physics, a Feynman diagram is a pictorial representation of the mathematical expressions describing the behavior and interaction of subatomic particles. The scheme is named after America ...
*
Angular momentum diagrams (quantum mechanics) In quantum mechanics and its applications to quantum many-particle systems, notably quantum chemistry, angular momentum diagrams, or more accurately from a mathematical viewpoint angular momentum graphs, are a diagrammatic method for representing ...


Notes


References


Sources

* * * (expanded, updated version of 't Hooft & Veltman, 1973, cited above) * *


External links


AMS article: "What's New in Mathematics: Finite-dimensional Feynman Diagrams"

Draw Feynman diagrams
explained by Flip Tanedo at Quantumdiaries.com
Drawing Feynman diagrams with FeynDiagram
C++ library that produces PostScript output.
Online Diagram Tool
A graphical application for creating publication ready diagrams.
JaxoDraw
A Java program for drawing Feynman diagrams. * {{Richard Feynman Concepts in physics Scattering theory Quantum field theory Diagrams Richard Feynman 1948 introductions