Quantum Field Theory

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Quantum field theory or QFT provides a theoretical framework for constructing ... In quantum field theory (QFT) the forces between particles are mediated by other ...
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quantum field theory ( ?kwänt?m ?f?ld ?th??r? ) ( quantum mechanics ) Quantum theory of physical systems possessing an infinite number of degrees of
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Quantum field theory (QFT) is a theoretical framework for constructing quantum mechanics models offield (physics) systems, or, equivalently, of Many-body problem. It is widely used in particle physics and condensed matter physics. Most theories in modern particle physics, including the Standard Model of elementary particles and their interactions, are formulated as Special relativity quantum field theories. In condensed matter physics, quantum field theories are used in many circumstances, especially those where the number of particles is allowed to fluctuate—for example, in the BCS theory of superconductivity.

History Quantum field theory originated in the 1920s from the problem of creating a quantum mechanics of the electromagnetic field. In 1926, Max Born, Pascual Jordan, and Werner Heisenberg constructed such a theory by expressing the field's internal Degrees of freedom (physics and chemistry) as an infinite set of harmonic oscillators and employing the usual procedure for quantizing those oscillators (canonical quantization). This theory assumed that no source (vector calculus) were present, and would today be called a free field theory. The first reasonably complete theory of quantum electrodynamics, which included both the electromagnetic field and electrically charged matter (specifically, electrons) as quantum mechanical objects, was created by Paul Dirac in 1927. This quantum field theory could be used to model important processes such as the emission of a photon by an electron dropping into a quantum state of lower energy, a process in which the number of particles changes — one atom in the initial state becomes an atom plus a photon in the final state. It is now understood that the ability to describe such processes is one of the most important features of quantum field theory.

It was obvious from the beginning that a proper quantum treatment of the electromagnetic field had to somehow incorporate Albert Einstein relativity theory, which had after all grown out of the study of classical electromagnetism. This need to put together relativity and quantum mechanics was the second major motivation in the development of quantum field theory. Jordan and Wolfgang Pauli showed in 1928 that quantum fields could be made to behave in the way predicted by special relativity during Covariance and contravariance of vectors (specifically, they showed that the field commutators were Lorentz invariant), and in 1933 Niels Bohr and Leon Rosenfeld showed that this result could be interpreted as a limitation on the ability to measure fields at space-like separations, exactly as required by relativity. A further boost for quantum field theory came with the discovery of the Dirac equation, a single-particle equation obeying both relativity and quantum mechanics, when it was shown that several of its undesirable properties (such as negative-energy states) could be eliminated by reformulating the Dirac equation as a quantum field theory. This work was performed by Wendell Furry, Robert Oppenheimer, Vladimir Fock, and others.

The third thread in the development of quantum field theory was the need to handle the statistics of many-particle systems consistently and with ease. In 1927, Jordan tried to extend the canonical quantization of fields to the many-body wavefunctions of identical particles, a procedure that is sometimes called second quantization. In 1928, Jordan and Eugene Wigner found that the quantum field describing electrons, or other fermions, had to be expanded using anti-commuting creation and annihilation operators due to the Pauli exclusion principle. This thread of development was incorporated into many-body theory, and strongly influenced condensed matter physics and nuclear physics.

Despite its early successes, quantum field theory was plagued by several serious theoretical difficulties. Many seemingly-innocuous physical quantities, such as the energy shift of electron states due to the presence of the electromagnetic field, gave infinity — a nonsensical result — when computed using quantum field theory. This "divergence problem" was solved during the 1940s by Bethe, Sin-Itiro Tomonaga, Julian Schwinger, Richard Feynman, and Freeman Dyson, through the procedure known as renormalization. This phase of development culminated with the construction of the modern theory of quantum electrodynamics (QED). Beginning in the 1950s with the work of Chen Ning Yang and Robert Mills (physicist), QED was generalized to a class of quantum field theories known as gauge theory. The 1960s and 1970s saw the formulation of a gauge theory now known as the Standard Model of particle physics, which describes all known elementary particles and the interactions between them. This effort was carried out by Martinus Veltman, Gerard 't Hooft, Frank Wilczek, David Gross, David Politzer and others.

Also during the 1970s, parallel developments in the study of phase transitions in condensed matter physics led Kenneth Wilson (following work byMichael Fisher and Leo Kadanoff) to a set of ideas and methods known as the renormalization group. By providing a better physical understanding of the renormalization procedure invented in the 1940s, the renormalization group sparked what has been called the "grand synthesis" of theoretical physics, uniting the quantum field theoretical techniques used in particle physics and condensed matter physics into a single theoretical framework.

The study of quantum field theory is alive and flourishing, as are applications of this method to many physical problems. It remains one of the most vital areas of theoretical physics today, providing a common language to many branches of physics.

Principles of quantum field theory Classical fields and quantum fields Quantum mechanics, in its most general formulation, is a theory of abstract operators (observables) acting on an abstract Hilbert space, where the observables represent physically-observable quantities and the Hilbert space represents the possible states of the system under study. Furthermore, each observable correspondence principle, in a technical sense, to the classical idea of a degree of freedom. For instance, the fundamental observables associated with the motion of a single quantum mechanical particle are the position and momentum operators \hat{x} and \hat{p}. Ordinary quantum mechanics deals with systems such as this, which possess a small set of degrees of freedom.

(It is important to note, at this point, that this article does not use the word "particle" in the context of wave–particle duality. In quantum field theory, "particle" is a generic term for any discrete quantum mechanical entity, such as an electron. Therefore, "particles" can behave like particle or wave under different experimental conditions.)

A quantum field is an quantum mechanical system containing a large, and possibly infinite, number of degrees of freedom. This is not as exotic a situation as one might think: a Field (physics), such as the classical electromagnetic field, contains a set of degrees of freedom at each point of space. In the case of the electromagnetic field, there are two vectors — the electric field and the magnetic field — that can in principle take on distinct values for each position r. When the field as a whole is considered as a quantum mechanical system, its observables form an uncountable set, because r is continuous.

Furthermore, the degrees of freedom in a quantum field are arranged in "repeated" sets. For example, the degrees of freedom in an electromagnetic field can be grouped according to the position r, with exactly two vectors for each r. Note that r is therefore an ordinary number that "indexes" the observables; it is not to be confused with the position operator \hat{x} encountered in ordinary quantum mechanics, which is an observable. (Thus, ordinary quantum mechanics is sometimes referred to as "zero-dimensional quantum field theory", because it contains only a single set of observables.) It is also important to note that there is nothing special about r because, as it turns out, there is generally more than one way of indexing the degrees of freedom in the field.

In the following sections, we will show how these ideas can be used to construct a quantum mechanical theory with the desired properties. We will begin by discussing single-particle quantum mechanics and the associated theory of many-particle quantum mechanics. Then, by finding a way to index the degrees of freedom in the many-particle problem, we will construct a quantum field and study its implications.

Single-particle and many-particle quantum mechanics In ordinary quantum mechanics, the time-dependent Schrödinger equation describing the motion of a single non-relativistic particle is

\left \frac{|\mathbf{p}|^2}{2m} + V(\mathbf{r}) \right |\psi(t)\rang = i \hbar \frac{\partial}{\partial t} |\psi(t)\rang,

where m is the particle'smass, V is the applied potential, and ] (we are using bra-ket notation).

We wish to consider how this problem generalizes to N particles. There are two motivations for studying the many-particle problem. The first is a straightforward need in condensed matter physics, where typically the number of particles is on the order of Avogadro's number (approximately 1023). The second motivation for the many-particle problem arises from particle physics and the desire to incorporate the effects of special relativity. If one attempts to include the relativistic rest energy into the above equation, the result is either the Klein-Gordon equation or the Dirac equation. However, these equations have many unsatisfactory qualities; for instance, they possess energy eigenvalues which extend to –∞, so that there seems to be no easy definition of a ground state. It turns out that such inconsistencies arise from neglecting the possibility of dynamically creating or destroying particles, which is a crucial aspect of relativity. Albert Einstein famous E=mc^2 predicts that sufficiently massive particles can decay into several lighter particles, and sufficiently energetic particles can combine to form massive particles. For example, an electron and a positron can annihilate each other to create photons. Thus, a consistent relativistic quantum theory must be formulated as a many-particle theory.

Let us therefore consider a system with N particles. We will furthermore, assume that the particles are identical particles. As described in the article on identical particles, this implies that the state of the entire system must be either symmetric (bosons) or antisymmetric (fermions) when the coordinates of its constituent particles are exchanged. These multi-particle states are rather complicated to write. For example, the general quantum state of a system of N bosons is written as

|\phi_1 \cdots \phi_N \rang = \sqrt{\frac{\prod_j N_j!}{N!--> \sum_{p\in S_N} |\phi_{p(1)}\rang \cdots |\phi_{p(N)} \rang,

where |\phi_i\rang are the single-particle states, N_j is the number of particles occupying state j, and the sum is taken over all possible permutations p acting on N elements. In general, this is a sum of N! (N factorial) distinct terms, which quickly becomes unmanageable as N increases.

Canonical quantization The way to simplify the many-particle problem is to turn it into a quantum field theory. The method we will present, which basically involves choosing a way to index the quantum mechanical degrees of freedom, is called canonical quantization or second quantization. It uses a Hamiltonian (quantum mechanics) formulation of the quantum mechanics. Several other approaches exist, such as the Feynman path integralsAbraham Pais, Inward Bound: Of Matter and Forces in the Physical World ISBN 0198519974. Pais recounts how his astonishment at the rapidity with which Feynman could calculate using his method. Feynman's method is now part of the standard methods for physicists., which uses a Lagrangian formulation. For an overview, see the article on quantization (physics).

Canonical quantization for bosons Suppose we have a system of N bosons which can occupy mutually orthogonal single-particle states |\phi_1\rang, |\phi_2\rang, |\phi_3\rang, and so on. The usual method of denoting a multi-particle state is to assign a state to each particle and then impose exchange symmetry. In the second quantized approach, we simply list the number of particles in each of the single-particle states. For a given set of such occupation numbers, it is understood that the corresponding multi-particle quantum state is the symmetrized combination of the indicated single-particle states.

To be specific, suppose that N=3, with one particle in state |\phi_1\rang and two in state|\phi_2\rang. The normal way of writing the wavefunction is

\frac{1}{\sqrt{3--> \left[ |\phi_1\rang |\phi_2\rang |\phi_2\rang + |\phi_2\rang |\phi_1\rang |\phi_2\rang + |\phi_2\rang|\phi_2\rang |\phi_1\rang \right].

In second quantized form, we write this as

|1, 2, 0, 0, 0, \cdots \rangle,

which means "one particle in state 1, two particles in state 2, and zero particles in all the other states."

Though the difference is entirely notational, the latter form makes it easy for us to define creation and annihilation operators, which add and subtract particles from multi-particle states. These creation and annihilation operators are very similar to those defined for the quantum harmonic oscillator, which added and subtracted energy quanta. However, these operators literally create and annihilate particles with a given quantum state. The bosonic annihilation operator a_2 and creation operator a_2^\dagger have the following effects:

a_2 | N_1, N_2, N_3, \cdots \rangle = \sqrt{N_2} \mid N_1, (N_2 - 1), N_3, \cdots \rangle, a_2^\dagger | N_1, N_2, N_3, \cdots \rangle = \sqrt{N_2 + 1} \mid N_1, (N_2 + 1), N_3, \cdots \rangle.

We may well ask whether these are operators in the usual quantum mechanical sense, i.e. linear operators acting on an abstract Hilbert space. In fact, the answer is yes: they are operators acting on a kind of expanded Hilbert space, known as a Fock space, composed of the space of a system with no particles (the so-called vacuum state), plus the space of a 1-particle system, plus the space of a 2-particle system, and so forth. Furthermore, the creation and annihilation operators are indeed Hermitian adjoint, which justifies the way we have written them.

The bosonic creation and annihilation operators obey the commutator

\left , a_j \right = 0 \quad,\quad\left , a_j^\dagger \right = 0 \quad,\quad\left , a_j^\dagger \right = \delta_{ij},

where \delta stands for the Kronecker delta. These are precisely the relations obeyed by the "ladder operators" for an infinite set of independent quantum harmonic oscillators, one for each single-particle state. Adding or removing bosons from each state is therefore analogous to exciting or de-exciting a quantum of energy in a harmonic oscillator.

The final step toward obtaining a quantum field theory is to re-write our original N-particle Hamiltonian in terms of creation and annihilation operators acting on a Fock space. For instance, the Hamiltonian of a field of free (non-interacting) bosons is

H = \sum_k E_k \, a^\dagger_k \,a_k,

where E_k is the energy of the k-th single-particle energy eigenstate. Note that

a_k^\dagger\,a_k|\cdots, N_k, \cdots \rangle=N_k| \cdots, N_k, \cdots \rangle.

Canonical quantization for fermions It turns out that the creation and annihilation operators for fermions must be defined differently, in order to satisfy the Pauli exclusion principle. For fermions, the occupation numbers N_i can only take on the value 0 or 1, since particles cannot share quantum states. We then define the fermionic annihilation operators c and creation operators c^\dagger by

c_j | N_1, N_2, \cdots, N_j = 0, \cdots \rangle = 0 c_j | N_1, N_2, \cdots, N_j = 1, \cdots \rangle = (-1)^{(N_1 + \cdots + N_{j-1})} | N_1, N_2, \cdots, N_j = 0, \cdots \rangle c_j^\dagger | N_1, N_2, \cdots, N_j = 0, \cdots \rangle = (-1)^{(N_1 + \cdots + N_{j-1})} | N_1, N_2, \cdots, N_j = 1, \cdots \rangle c_j^\dagger | N_1, N_2, \cdots, N_j = 1, \cdots \rangle = 0

The fermionic creation and annihilation operators obey an anticommutator,

\left\{c_i , c_j \right\} = 0 \quad,\quad\left\{c_i^\dagger , c_j^\dagger \right\} = 0 \quad,\quad\left\{c_i , c_j^\dagger \right\} = \delta_{ij}

One may notice from this that applying a fermionic creation operator twice gives zero, so it is impossible for the particles to share single-particle states, in accordance with the exclusion principle.

Significance of creation and annihilation operators When we re-write a Hamiltonian using a Fock space and creation and annihilation operators, as in the previous example, the symbol N, which stands for the total number of particles, drops out. This means that the Hamiltonian is applicable to systems with any number of particles. Of course, in many common situations N is a physically important and perfectly well-defined quantity. For instance, if we are describing a gas of atoms sealed in a box, the number of atoms had better remain a constant at all times. This is certainly true for the above Hamiltonian. Viewing the Hamiltonian as the generator of time evolution, we see that whenever an annihilation operator a_k destroys a particle during an infinitesimal time step, the creation operator a_k^\dagger to the left of it instantly puts it back. Therefore, if we start with a state of N non-interacting particles then we will always have N particles at a later time.

On the other hand, it is often useful to consider quantum states where the particle number is ill-defined, i.e. linear superpositions of vectors from the Fock space that possess different values of N. For instance, it may happen that our bosonic particles can be created or destroyed by interactions with a field of fermions. Denoting the fermionic creation and annihilation operators by c_k^\dagger and c_k, we could add a "potential energy" term to our Hamiltonian such as:

V = \sum_{k,q} V_q (a_q + a_{-q}^\dagger) c_{k+q}^\dagger c_k

This describes processes in which a fermion in state k either absorbs or emits a boson, thereby being kicked into a different eigenstate k+q. In fact, this is the expression for the interaction between phonons and conduction electrons in a solid. The interaction between photons and electrons is treated in a similar way; it is a little more complicated, because the role of spin (physics) must be taken into account. One thing to notice here is that even if we start out with a fixed number of bosons, we will generally end up with a superposition of states with different numbers of bosons at later times. On the other hand, the number of fermions is conserved in this case.

In condensed matter physics, states with ill-defined particle numbers are also very important for describing the various superfluids. Many of the defining characteristics of a superfluid arise from the notion that its quantum state is a superposition of states with different particle numbers.

Field operators We can now define field operators that create or destroy a particle at a particular point in space. In particle physics, these are often more convenient to work with than the creation and annihilation operators, because they make it easier to formulate theories that satisfy the demands of relativity.

Single-particle states are usually enumerated in terms of their momentum (as in the particle in a box problem.) We can construct field operators by applying the Fourier transform to the creation and annihilation operators for these states. For example, the bosonic field annihilation operator \phi(\mathbf{r}) is

\phi(\mathbf{r}) \ \stackrel{\mathrm{def-->{=}\ \sum_{j} e^{i\mathbf{k}_j\cdot \mathbf{r--> a_{j}

The bosonic field operators obey the commutation relation

\left , \phi(\mathbf{r'}) \right = 0 \quad,\quad\left , \phi^\dagger(\mathbf{r'}) \right = 0 \quad,\quad\left , \phi^\dagger(\mathbf{r'}) \right = \delta^3(\mathbf{r} - \mathbf{r'})

where \delta(x) stands for the Dirac delta function. As before, the fermionic relations are the same, with the commutators replaced by anticommutators.

It should be emphasized that the field operator is not the same thing as a single-particle wavefunction. The former is an operator acting on the Fock space, and the latter is just a scalar field. However, they are closely related, and are indeed commonly denoted with the same symbol. If we have a Hamiltonian with a space representation, say

H = - \frac{\hbar^2}{2m} \sum_i \nabla_i^2 + \sum_{i < j} U(|\mathbf{r}_i - \mathbf{r}_j|)

where the indices i and j run over all particles, then the field theory Hamiltonian is

H = - \frac{\hbar^2}{2m} \int d^3\!r \; \phi(\mathbf{r})^\dagger \nabla^2 \phi(\mathbf{r}) + \int\!d^3\!r \int\!d^3\!r' \; \phi(\mathbf{r})^\dagger \phi(\mathbf{r}')^\dagger U(|\mathbf{r} - \mathbf{r}'|) \phi(\mathbf{r'}) \phi(\mathbf{r})

This looks remarkably like an expression for the expectation value of the energy, with \phi playing the role of the wavefunction. This relationship between the field operators and wavefunctions makes it very easy to formulate field theories starting from space-projected Hamiltonians.

Field quantization The essential difference between an ordinary system of particles and the electromagnetic field is the number of dynamical degrees of freedom. For a system of N particles, there are 3N coordinate variables corresponding to the position of each particle, and 3N conjugate momentum variables. One formulates a Hamiltonian mechanics using these variables, and obtains a quantum theory by turning the coordinate and position variables into quantum operators, and postulating Canonical commutation relation between them such as

\left q_i , p_j \right =i \delta_{ij}

For an electromagnetic field, the analogue of the coordinate variables are the values of the electrical potential \phi(\mathbf{x}) and the vector potential \mathbf{A}(\mathbf{x}) at every point \mathbf{x}. This is an uncountable set of variables, because \mathbf{x} is continuous. This prevents us from postulating the same commutation relation as before. The way out is to replace the Kronecker delta with a Dirac delta function. This ends up giving us a commutation relation exactly like the one for field operators! We therefore end up treating "fields" and "particles" in the same way, using the apparatus of quantum field theory. Only by accident electrons were not regarded as Louis, 7th duc de Broglie waves and photons governed by geometrical optics were not the dominant theory when QFT was developed.

Path integral methods The axiomatic approach There have been many attempts to put quantum field theory on a firm mathematical footing by formulating a set of axioms for it. These attempts fall into two broad classes.

The Wightman axioms (most notably the Wightman axioms, Osterwalder-Schrader theorem, and Haag-Kastler systems) tried to formalize the physicists' notion of an "operator-valued field" within the context of functional analysis. These axioms enjoyed limited success. It was possible to prove that any QFT satisfying these axioms satisfied certain general theorems, such as the spin-statistics theorem and the PCT theorems. Unfortunately, it proved extraordinarily difficult to show that any realistic field theory (e.g. quantum chromodynamics) satisfied these axioms. Most of the theories which could be treated with these analytic axioms were physically trivial: restricted to low-dimensions and lacking in interesting dynamics. Constructive quantum field theory is the construction of theories which satisfy one of these sets of axioms. Important work was done in this area in the 1970s by Segal, Glimm, Jaffe and others.

In the 1980s, a Topological quantum field theory were proposed. These axioms (associated most closely with Atiyah and Segal, and notably expanded upon by Witten, Borcherds, and Kontsevich) are more geometric in nature, and more closely resemble the path integrals of physics. They have not been exceptionally useful to physicists, as it is still extraordinarily difficult to show that any realistic QFTs satisfy these axioms, but have found many applications in mathematics, particularly in representation theory, algebraic topology, and geometry.

Finding the proper axioms for quantum field theory is still an open and difficult problem in mathematics. In fact, one of the Millennium Prize Problems offers $1,000,000 to anyone who proves the existence of a Yang-Mills existence and mass gap. It seems likely that we have not yet understood the underlying structures which permit the Feynman path integrals to exist.

Renormalization Some of the problems and phenomena eventually addressed by renormalization actually appeared earlier in the classical electrodynamics of point particles in the 19th century and early 20th century. The basic problem is that the observable properties of an interacting particle cannot be entirely separated from the field that mediates the interaction. The standard classical example is the energy of a charged particle. To cram a finite amount of charge into a single point requires an infinite amount of energy; this manifests itself as the infinite energy of the particle's electric field. The energy density grows to infinity as one gets close to the charge.

A single particle state in quantum field theory incorporates within it multiparticle states. This is most simply demonstrated by examining the evolution of a single particle state in the interaction picture— :|\psi(t)\rangle = e^{iH_It} |\psi(0)\rangle = \left H_I^2t^2 -\frac i{3!}H_I^3t^3 + \frac1{4!}H_I^4t^4 + \cdots\right |\psi(0)\rangle. Taking the overlap with the initial state, one retains the even powers of HI. These terms are responsible for changing the number of particles during propagation, and are therefore quintessentially a product of quantum field theory. Corrections such as these are incorporated into wave function renormalization and mass renormalization. Similar corrections to the interaction Hamiltonian (quantum mechanics), HI, include vertex renormalization, or, in modern language, effective field theory.

Gauge theories A gauge theory is a theory which admits a Symmetry in physics with a local parameter. For example, in every quantum mechanics theory the global Phase (waves) of the wave function is arbitrary and does not represent something physical, so the theory is invariant under a global change of phases (adding a constant to the phase of all wave functions, everywhere); this is a global symmetry. In quantum electrodynamics, the theory is also invariant under a local change of phase, that is - one may shift the phase of all wave functions so that in every point in space-time the shift is different. This is a local symmetry. However, in order for a well-defined derivative operator to exist, one must introduce a new field (physics), the gauge field, which also transforms in order for the local change of variables (the phase in our example) not to affect the derivative. In quantum electrodynamics this gauge field is the electromagnetic field. The change of local change of variables is termed gauge transformation.

In quantum field theory the excitations of fields represent Elementary particle. The particle associated with excitations of the gauge field is the gauge boson, which is the photon in the case of quantum electrodynamics.

The Degrees of freedom (physics and chemistry) in quantum field theory are local fluctuations of the fields. The existence of a gauge symmetry reduces the number of degrees of freedom, simply because some fluctuations of the fields can be transformed to zero by gauge transformations, so they are equivalent to having no fluctuations at all, and they therefore have no physical meaning. Such fluctuations are usually called "non-physical degrees of freedom" or gauge artifacts; usually some of them have a negative norm (mathematics), making them inadequate for a consistent theory. Therefore, if a classical field theory has a gauge symmetry, then its quantized version (i.e. the corresponding quantum field theory) will have this symmetry as well. In other words, a gauge symmetry cannot have a quantum Anomaly (physics). If a gauge symmetry is Gauge anomaly (i.e. not kept in the quantum theory) then the theory is non-consistent: for example, in quantum electrodynamics, had there been a gauge anomaly, this would require the appearance of photons with Longitudinal wave polarization and polarization in the time direction, the latter having a negative norm (mathematics), rendering the theory inconsistent; another possibility would be for these photons to appear only in intermediate processes but not in the final products of any interaction, making the theory non unitarity and again inconsistent (see optical theorem).

In general, the gauge transformations of a theory consist several different transformations, which may not be commutative. These transformations are together described by a mathematical object known as a gauge group. Infinitesimal gauge transformations are the gauge group Generator (mathematics). Therefore the number of gauge bosons is the group Dimension (vector space) (i.e. number of generators forming a Basis (linear algebra)).

All the fundamental interactions in nature are described by Gauge theory. These are:

Quantum electrodynamics, whose gauge transformation is a local change of phase, so that the gauge group is U(1). The gauge boson is the photon.
Quantum chromodynamics, whose gauge group is SU(3). The gauge bosons are eight gluons.
The Weak interaction, whose gauge group is U(1)\times SU(2) (a direct product of U(1) and SU(2)).
Gravity, whose classical theory is general relativity, admits the equivalence principle which is a form of gauge symmetry.

Supersymmetry Supersymmetry assumes that every fundamental fermion has a superpartner which is a boson and vice versa. It was introduced in order to solve the so-called Hierarchy Problem, that is, to explain why particles not protected by any symmetry (like the Higgs boson) do not receive radiative corrections to its mass driving it to the larger scales (GUT, Planck...). It was soon realized that supersymmetry has other interesting properties: its gauged version is an extension of general relativity (Supergravity), and it is a key ingredient for the consistency of string theory.

The way supersymmetry protects the hierarchies is the following: since for every particle there is a superpartner with the same mass, any loop in a radiative correction is cancelled by the loop corresponding to its superpartner, rendering the theory UV finite.

Since no superpartners have yet been observed, if supersymmetry exists it must be broken (through a so-called soft term, which breaks supersymmetry without ruining its helpful features). The simplest models of this breaking require that the energy of the superpartners not be too high; in these cases, supersymmetry is expected to be observed by experiments at the Large Hadron Collider.

See also

List of quantum field theories
Feynman path integral
Quantum chromodynamics
Quantum electrodynamics
Schwinger-Dyson equation
Relationship between string theory and quantum field theory
Abraham-Lorentz force
Photon polarization
Theoretical and experimental justification for the Schrödinger equation
Invariance mechanics

Notes Suggested reading

Wilczek, Frank ; Quantum Field Theory, Review of Modern Physics 71 (1999) S85-S95. Review article written by a master of Q.C.D., Nobel laureate 2003. Full text available at : hep-th/9803075

Ryder, Lewis H. ; Quantum Field Theory (Cambridge University Press, 1985), 0-521-33859-X. Introduction to relativistic Q.F.T. for particle physics.

Zee, Anthony ; Quantum Field Theory in a Nutshell, Princeton University Press (2003) 0-691-01019-6.
Peskin, M and Schroeder, D. ;An Introduction to Quantum Field Theory (Westview Press, 1995) 0-201-50397-2

Weinberg, Steven ; The Quantum Theory of Fields (3 volumes) Cambridge University Press (1995). A monumental treatise on Q.F.T. written by a leading expert, Nobel laureate 1979.

Loudon, Rodney ; The Quantum Theory of Light (Oxford University Press, 1983), 0-19-851155-8

Paul Frampton , Gauge Field Theories, Frontiers in Physics, Addison-Wesley (1986), Second Edition, Wiley (2000).

External links

Siegel, Warren ; Fields (also available from arXiv:hep-th/9912205)
't Hooft, Gerard ; The Conceptual Basis of Quantum Field Theory, Handbook of the Philosophy of Science, Elsevier (to be published). Review article written by a master of gauge theories, laureate 1999. Full text available in .
Srednicki, Mark ; Quantum Field Theory
Kuhlmann, Meinard ; Quantum Field Theory, Stanford Encyclopedia of Philosophy
Quantum field theory textbooks: a list with links to amazon.com

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