**Symmetries in quantum mechanics** describe features of spacetime and particles which are unchanged under some transformation, in the context of quantum mechanics, relativistic quantum mechanics and quantum field theory, and with applications in the mathematical formulation of the standard model and condensed matter physics. In general, symmetry in physics, invariance, and conservation laws, are fundamentally important constraints for formulating physical theories and models. In practice, they are powerful methods for solving problems and predicting what can happen. While conservation laws do not always give the answer to the problem directly, they form the correct constraints and the first steps to solving a multitude of problems.

- Notation
- Symmetry transformations on the wavefunction in non-relativistic quantum mechanics
- Continuous symmetries
- Overview of Lie group theory
- Momentum and energy as generators of translation and time evolution, and rotation
- Angular momentum as the generator of rotations
- Conserved quantities in the Quantum Harmonic Oscillator
- Lorentz group in relativistic quantum mechanics
- Pure rotations in spacetime
- Pure boosts in spacetime
- Combining boosts and rotations
- Transformations of spinor wavefunctions in relativistic quantum mechanics
- Real irreducible representations and spin
- Relativistic wave equations
- The Poincaré group in relativistic quantum mechanics and field theory
- Symmetries in quantum field theory and particle physics
- Unitary groups in quantum field theory
- Matter and antimatter
- Discrete spacetime symmetries
- C, P, T symmetries
- Gauge theory
- The strong (color) interaction
- The weak and electromagnetic interactions
- Supersymmetry
- Exchange symmetry or permutation symmetry
- See also
- Footnotes
- References
- Further reading
- External links

This article outlines the connection between the classical form of continuous symmetries as well as their quantum operators, and relates them to the Lie groups, and relativistic transformations in the Lorentz group and Poincaré group.

The notational conventions used in this article are as follows. Boldface indicates vectors, four vectors, matrices, and vectorial operators, while quantum states use bra–ket notation. Wide hats are for operators, narrow hats are for unit vectors (including their components in tensor index notation). The summation convention on the repeated tensor indices is used, unless stated otherwise. The Minkowski metric signature is (+−−−).

Generally, the correspondence between continuous symmetries and conservation laws is given by Noether's theorem.

The form of the fundamental quantum operators, for example energy as a partial time derivative and momentum as a spatial gradient, becomes clear when one considers the initial state, then changes one parameter of it slightly. This can be done for displacements (lengths), durations (time), and angles (rotations). Additionally, the invariance of certain quantities can be seen by making such changes in lengths and angles, illustrating conservation of these quantities.

In what follows, transformations on only one-particle wavefunctions in the form:

are considered, where denotes a unitary operator. Unitarity is generally required for operators representing transformations of space, time, and spin, since the norm of a state (representing the total probability of finding the particle somewhere with some spin) must be invariant under these transformations. The inverse is the Hermitian conjugate . The results can be extended to many-particle wavefunctions. Written in Dirac notation as standard, the transformations on quantum state vectors are:

Now, the action of changes *ψ*(**r**, *t*) to *ψ*(**r**′, *t*′), so the inverse changes *ψ*(**r**′, *t*′) back to *ψ*(**r**, *t*), so an operator invariant under satisfies:

and thus:

for any state *ψ*. Quantum operators representing observables are also required to be Hermitian so that their eigenvalues are real numbers, i.e. the operator equals its Hermitian conjugate, .

Following are the key points of group theory relevant to quantum theory, examples are given throughout the article. For an alternative approach using matrix groups, see the books of Hall^{ [1] }^{ [2] }

Let *G* be a * Lie group *, which is a group that locally is parameterized by a finite number *N* of real continuously varying parameters *ξ*_{1}, *ξ*_{2}, ... *ξ*_{N}. In more mathematical language, this means that *G* is a smooth manifold that is also a group, for which the group operations are smooth.

- the
*dimension of the group*,*N*, is the number of parameters it has. - the
*group elements*,*g*, in*G*are functions of the parameters:

- and all parameters set to zero returns the
*identity element*of the group: - Group elements are often matrices which act on vectors, or transformations acting on functions.

- The
*generators of the group*are the partial derivatives of the group elements with respect to the group parameters with the result evaluated when the parameter is set to zero:

- In the language of manifolds, the generators are the elements of the tangent space to
*G*at the identity. The generators are also known as infinitesimal group elements or as the elements of the Lie algebra of*G*. (See the discussion below of the commutator.) - One aspect of generators in theoretical physics is they can be constructed themselves as operators corresponding to symmetries, which may be written as matrices, or as differential operators. In quantum theory, for unitary representations of the group, the generators require a factor of
*i*: - The generators of the group form a vector space, which means linear combinations of generators also form a generator.

- The generators (whether matrices or differential operators) satisfy the
*commutation relations*:

- where
*f*are the (basis dependent)_{abc}*structure constants*of the group. This makes, together with the vector space property, the set of all generators of a group a Lie algebra. Due to the antisymmetry of the bracket, the structure constants of the group are antisymmetric in the first two indices.

- The
*representations of the group*then describe the ways that the group*G*(or its Lie algebra) can act on a vector space. (The vector space might be, for example, the space of eigenvectors for a Hamiltonian having*G*as its symmetry group.) We denote the representations using a capital*D*. One can then differentiate*D*to obtain a representation of the Lie algebra, often also denoted by*D*. These two representations are related as follows:

*without*summation on the repeated index*j*. Representations are linear operators that take in group elements and preserve the composition rule:

A representation which cannot be decomposed into a direct sum of other representations, is called *irreducible*. It is conventional to label irreducible representations by a superscripted number *n* in brackets, as in *D*^{(n)}, or if there is more than one number, we write *D*^{(n, m, ... )}.

There is an additional subtlety that arises in quantum theory, where two vectors that differ by multiplication by a scalar represent the same physical state. Here, the pertinent notion of representation is a projective representation, one that only satisfies the composition law up to a scalar. In the context of quantum mechanical spin, such representations are called spinorial.

The space translation operator acts on a wavefunction to shift the space coordinates by an infinitesimal displacement Δ**r**. The explicit expression can be quickly determined by a Taylor expansion of *ψ*(**r** + Δ**r**, *t*) about **r**, then (keeping the first order term and neglecting second and higher order terms), replace the space derivatives by the momentum operator . Similarly for the time translation operator acting on the time parameter, the Taylor expansion of *ψ*(**r**, *t* + Δ*t*) is about *t*, and the time derivative replaced by the energy operator .

Name Translation operator Time translation/evolution operator Action on wavefunction Infinitesimal operator Finite operator Generator Momentum operator Energy operator

The exponential functions arise by definition as those limits, due to Euler, and can be understood physically and mathematically as follows. A net translation can be composed of many small translations, so to obtain the translation operator for a finite increment, replace Δ**r** by Δ**r**/*N* and Δ*t* by Δ*t*/*N*, where *N* is a positive non-zero integer. Then as *N* increases, the magnitude of Δ**r** and Δ*t* become even smaller, while leaving the directions unchanged. Acting the infinitesimal operators on the wavefunction *N* times and taking the limit as *N* tends to infinity gives the finite operators.

Space and time translations commute, which means the operators and generators commute.

Commutators Operators Generators

For a time-independent Hamiltonian, energy is conserved in time and quantum states are stationary states: the eigenstates of the Hamiltonian are the energy eigenvalues *E*:

and all stationary states have the form

where *t*_{0} is the initial time, usually set to zero since there is no loss of continuity when the initial time is set.

An alternative notation is .

The rotation operator acts on a wavefunction to rotate the spatial coordinates of a particle by a constant angle Δ*θ*:

where **r′** are the rotated coordinates about an axis defined by a unit vector through an angular increment Δ*θ*, given by:

where is a rotation matrix dependent on the axis and angle. In group theoretic language, the rotation matrices are group elements, and the angles and axis are the parameters, of the three-dimensional special orthogonal group, SO(3). The rotation matrices about the standard Cartesian basis vector through angle Δ*θ*, and the corresponding generators of rotations **J** = (*J _{x}*,

More generally for rotations about an axis defined by , the rotation matrix elements are:^{ [3] }

where *δ _{ij}* is the Kronecker delta, and

It is not as obvious how to determine the rotational operator compared to space and time translations. We may consider a special case (rotations about the *x*, *y*, or *z*-axis) then infer the general result, or use the general rotation matrix directly and tensor index notation with *δ _{ij}* and

Rotation about Rotation about Action on wavefunction Infinitesimal operator Infinitesimal rotations Same Finite rotations Same Generator *z*-component of the angular momentum operatorFull angular momentum operator .

The *z*-component of angular momentum can be replaced by the component along the axis defined by , using the dot product .

Again, a finite rotation can be made from many small rotations, replacing Δ*θ* by Δ*θ*/*N* and taking the limit as *N* tends to infinity gives the rotation operator for a finite rotation.

Rotations about the *same* axis do commute, for example a rotation through angles *θ*_{1} and *θ*_{2} about axis *i* can be written

However, rotations about *different* axes do not commute. The general commutation rules are summarized by

In this sense, orbital angular momentum has the common sense properties of rotations. Each of the above commutators can be easily demonstrated by holding an everyday object and rotating it through the same angle about any two different axes in both possible orderings; the final configurations are different.

In quantum mechanics, there is another form of rotation which mathematically appears similar to the orbital case, but has different properties, described next.

All previous quantities have classical definitions. Spin is a quantity possessed by particles in quantum mechanics without any classical analogue, having the units of angular momentum. The spin vector operator is denoted . The eigenvalues of its components are the possible outcomes (in units of ) of a measurement of the spin projected onto one of the basis directions.

Rotations (of ordinary space) about an axis through angle *θ* about the unit vector in space acting on a multicomponent wave function (spinor) at a point in space is represented by:

However, unlike orbital angular momentum in which the *z*-projection quantum number *ℓ* can only take positive or negative integer values (including zero), the *z*-projection spin quantum number *s* can take all positive and negative half-integer values. There are rotational matrices for each spin quantum number.

Evaluating the exponential for a given *z*-projection spin quantum number *s* gives a (2*s* + 1)-dimensional spin matrix. This can be used to define a spinor as a column vector of 2*s* + 1 components which transforms to a rotated coordinate system according to the spin matrix at a fixed point in space.

For the simplest non-trivial case of *s* = 1/2, the spin operator is given by

where the Pauli matrices in the standard representation are:

The total angular momentum operator is the sum of the orbital and spin

and is an important quantity for multi-particle systems, especially in nuclear physics and the quantum chemistry of multi-electron atoms and molecules.

We have a similar rotation matrix:

The dynamical symmetry group of the *n* dimensional quantum harmonic oscillator is the special unitary group SU(*n*). As an example, the number of infinitesimal generators of the corresponding Lie algebras of SU(2) and SU(3) are three and eight respectively. This leads to exactly three and eight independent conserved quantities (other than the Hamiltonian) in these systems.

The two dimensional quantum harmonic oscillator has the expected conserved quantities of the Hamiltonian and the angular momentum, but has additional hidden conserved quantities of energy level difference and another form of angular momentum.

Following is an overview of the Lorentz group; a treatment of boosts and rotations in spacetime. Throughout this section, see (for example) T. Ohlsson (2011)^{ [4] } and E. Abers (2004).^{ [5] }

Lorentz transformations can be parametrized by rapidity *φ* for a boost in the direction of a three-dimensional unit vector , and a rotation angle *θ* about a three-dimensional unit vector defining an axis, so and are together six parameters of the Lorentz group (three for rotations and three for boosts). The Lorentz group is 6-dimensional.

The rotation matrices and rotation generators considered above form the spacelike part of a four-dimensional matrix, representing pure-rotation Lorentz transformations. Three of the Lorentz group elements and generators **J** = (*J*_{1}, *J*_{2}, *J*_{3}) for pure rotations are:

The rotation matrices act on any four vector **A** = (*A*_{0}, *A*_{1}, *A*_{2}, *A*_{3}) and rotate the space-like components according to

leaving the time-like coordinate unchanged. In matrix expressions, **A** is treated as a column vector.

A boost with velocity *c*tanh*φ* in the *x*, *y*, or *z* directions given by the standard Cartesian basis vector , are the boost transformation matrices. These matrices and the corresponding generators **K** = (*K*_{1}, *K*_{2}, *K*_{3}) are the remaining three group elements and generators of the Lorentz group:

The boost matrices act on any four vector **A** = (*A*_{0}, *A*_{1}, *A*_{2}, *A*_{3}) and mix the time-like and the space-like components, according to:

The term "boost" refers to the relative velocity between two frames, and is not to be conflated with momentum as the *generator of translations*, as explained below.

Products of rotations give another rotation (a frequent exemplification of a subgroup), while products of boosts and boosts or of rotations and boosts cannot be expressed as pure boosts or pure rotations. In general, any Lorentz transformation can be expressed as a product of a pure rotation and a pure boost. For more background see (for example) B.R. Durney (2011)^{ [6] } and H.L. Berk et al.^{ [7] } and references therein.

The boost and rotation generators have representations denoted *D*(**K**) and *D*(**J**) respectively, the capital *D* in this context indicates a group representation.

For the Lorentz group, the representations *D*(**K**) and *D*(**J**) of the generators **K** and **J** fulfill the following commutation rules.

Commutators Pure rotation Pure boost Lorentz transformation Generators Representations

In all commutators, the boost entities mixed with those for rotations, although rotations alone simply give another rotation. Exponentiating the generators gives the boost and rotation operators which combine into the general Lorentz transformation, under which the spacetime coordinates transform from one rest frame to another boosted and/or rotating frame. Likewise, exponentiating the representations of the generators gives the representations of the boost and rotation operators, under which a particle's spinor field transforms.

Transformation laws Pure boost Pure rotation Lorentz transformation Transformations Representations

In the literature, the boost generators **K** and rotation generators **J** are sometimes combined into one generator for Lorentz transformations **M**, an antisymmetric four-dimensional matrix with entries:

and correspondingly, the boost and rotation parameters are collected into another antisymmetric four-dimensional matrix **ω**, with entries:

The general Lorentz transformation is then:

with summation over repeated matrix indices *α* and *β*. The Λ matrices act on any four vector **A** = (*A*_{0}, *A*_{1}, *A*_{2}, *A*_{3}) and mix the time-like and the space-like components, according to:

In relativistic quantum mechanics, wavefunctions are no longer single-component scalar fields, but now 2(2*s* + 1) component spinor fields, where *s* is the spin of the particle. The transformations of these functions in spacetime are given below.

Under a proper orthochronous Lorentz transformation (**r**, *t*) → Λ(**r**, *t*) in Minkowski space, all one-particle quantum states *ψ _{σ}* locally transform under some representation

where *D*(Λ) is a finite-dimensional representation, in other words a (2*s* + 1)×(2*s* + 1) dimensional square matrix, and *ψ* is thought of as a column vector containing components with the (2*s* + 1) allowed values of *σ*:

The irreducible representations of *D*(**K**) and *D*(**J**), in short "irreps", can be used to build to spin representations of the Lorentz group. Defining new operators:

so **A** and **B** are simply complex conjugates of each other, it follows they satisfy the symmetrically formed commutators:

and these are essentially the commutators the orbital and spin angular momentum operators satisfy. Therefore, **A** and **B** form operator algebras analogous to angular momentum; same ladder operators, *z*-projections, etc., independently of each other as each of their components mutually commute. By the analogy to the spin quantum number, we can introduce positive integers or half integers, *a, b*, with corresponding sets of values *m* = *a*, *a* − 1, ... −*a* + 1, −*a* and *n* = *b*, *b* − 1, ... −*b* + 1, −*b*. The matrices satisfying the above commutation relations are the same as for spins *a* and *b* have components given by multiplying Kronecker delta values with angular momentum matrix elements:

where in each case the row number *m′n′* and column number *mn* are separated by a comma, and in turn:

and similarly for **J**^{(n)}.^{ [note 1] } The three **J**^{(m)} matrices are each (2*m* + 1)×(2*m* + 1) square matrices, and the three **J**^{(n)} are each (2*n* + 1)×(2*n* + 1) square matrices. The integers or half-integers *m* and *n* numerate all the irreducible representations by, in equivalent notations used by authors: *D*^{(m, n)} ≡ (*m*, *n*) ≡ *D*^{(m)}⊗*D*^{(n)}, which are each [(2*m* + 1)(2*n* + 1)]×[(2*m* + 1)(2*n* + 1)] square matrices.

Applying this to particles with spin *s*;

- left-handed (2
*s*+ 1)-component spinors transform under the real irreps*D*^{(s, 0)}, - right-handed (2
*s*+ 1)-component spinors transform under the real irreps*D*^{(0, s)}, - taking direct sums symbolized by ⊕ (see direct sum of matrices for the simpler matrix concept), one obtains the representations under which 2(2
*s*+ 1)-component spinors transform:*D*^{(m, n)}⊕*D*^{(n, m)}where*m*+*n*=*s*. These are also real irreps, but as shown above, they split into complex conjugates.

In these cases the *D* refers to any of *D*(**J**), *D*(**K**), or a full Lorentz transformation *D*(Λ).

In the context of the Dirac equation and Weyl equation, the Weyl spinors satisfying the Weyl equation transform under the simplest irreducible spin representations of the Lorentz group, since the spin quantum number in this case is the smallest non-zero number allowed: 1/2. The 2-component left-handed Weyl spinor transforms under *D*^{(1/2, 0)} and the 2-component right-handed Weyl spinor transforms under *D*^{(0, 1/2)}. Dirac spinors satisfying the Dirac equation transform under the representation *D*^{(1/2, 0)}⊕*D*^{(0, 1/2)}, the direct sum of the irreps for the Weyl spinors.

Space translations, time translations, rotations, and boosts, all taken together, constitute the Poincaré group. The group elements are the three rotation matrices and three boost matrices (as in the Lorentz group), and one for time translations and three for space translations in spacetime. There is a generator for each. Therefore, the Poincaré group is 10-dimensional.

In special relativity, space and time can be collected into a four-position vector **X** = (*ct*, −**r**), and in parallel so can energy and momentum which combine into a four-momentum vector **P** = (*E*/*c*, −**p**). With relativistic quantum mechanics in mind, the time duration and spatial displacement parameters (four in total, one for time and three for space) combine into a spacetime displacement Δ**X** = (*c*Δ*t*, −Δ**r**), and the energy and momentum operators are inserted in the four-momentum to obtain a four-momentum operator,

which are the generators of spacetime translations (four in total, one time and three space):

There are commutation relations between the components four-momentum **P** (generators of spacetime translations), and angular momentum **M** (generators of Lorentz transformations), that define the Poincaré algebra:^{ [10] }^{ [11] }

where *η* is the Minkowski metric tensor. (It is common to drop any hats for the four-momentum operators in the commutation relations). These equations are an expression of the fundamental properties of space and time as far as they are known today. They have a classical counterpart where the commutators are replaced by Poisson brackets.

To describe spin in relativistic quantum mechanics, the Pauli–Lubanski pseudovector

a Casimir operator, is the constant spin contribution to the total angular momentum, and there are commutation relations between **P** and **W** and between **M** and **W**:

Invariants constructed from **W**, instances of Casimir invariants can be used to classify irreducible representations of the Lorentz group.

Group theory is an abstract way of mathematically analyzing symmetries. Unitary operators are paramount to quantum theory, so unitary groups are important in particle physics. The group of *N* dimensional unitary square matrices is denoted U(*N*). Unitary operators preserve inner products which means probabilities are also preserved, so the quantum mechanics of the system is invariant under unitary transformations. Let be a unitary operator, so the inverse is the Hermitian adjoint , which commutes with the Hamiltonian:

then the observable corresponding to the operator is conserved, and the Hamiltonian is invariant under the transformation .

Since the predictions of quantum mechanics should be invariant under the action of a group, physicists look for unitary transformations to represent the group.

Important subgroups of each U(*N*) are those unitary matrices which have unit determinant (or are "unimodular"): these are called the special unitary groups and are denoted SU(*N*).

The simplest unitary group is U(1), which is just the complex numbers of modulus 1. This one-dimensional matrix entry is of the form:

in which *θ* is the parameter of the group, and the group is Abelian since one-dimensional matrices always commute under matrix multiplication. Lagrangians in quantum field theory for complex scalar fields are often invariant under U(1) transformations. If there is a quantum number *a* associated with the U(1) symmetry, for example baryon and the three lepton numbers in electromagnetic interactions, we have:

The general form of an element of a U(2) element is parametrized by two complex numbers *a* and *b*:

and for SU(2), the determinant is restricted to 1:

In group theoretic language, the Pauli matrices are the generators of the special unitary group in two dimensions, denoted SU(2). Their commutation relation is the same as for orbital angular momentum, aside from a factor of 2:

A group element of SU(2) can be written:

where *σ _{j}* is a Pauli matrix, and the group parameters are the angles turned through about an axis.

The two-dimensional isotropic quantum harmonic oscillator has symmetry group SU(2), while the symmetry algebra of the rational anisotropic oscillator is a nonlinear extension of u(2).^{ [12] }

The eight Gell-Mann matrices *λ _{n}* (see article for them and the structure constants) are important for quantum chromodynamics. They originally arose in the theory SU(3) of flavor which is still of practical importance in nuclear physics. They are the generators for the SU(3) group, so an element of SU(3) can be written analogously to an element of SU(2):

where *θ _{n}* are eight independent parameters. The

where the indices *a*, *b*, *c* take the values 1, 2, 3... 8. The structure constants *f _{abc}* are totally antisymmetric in all indices analogous to those of SU(2). In the standard colour charge basis (

the colour states are eigenstates of the *λ*_{3} and *λ*_{8} matrices, while the other matrices mix colour states together.

The eight gluons states (8-dimensional column vectors) are simultaneous eigenstates of the adjoint representation of SU(3) , the 8-dimensional representation acting on its own Lie algebra su(3), for the *λ*_{3} and *λ*_{8} matrices. By forming tensor products of representations (the standard representation and its dual) and taking appropriate quotients, protons and neutrons, and other hadrons are eigenstates of various representations of SU(3) of color. The representations of SU(3) can be described by a "theorem of the highest weight".^{ [13] }

In relativistic quantum mechanics, relativistic wave equations predict a remarkable symmetry of nature: that every particle has a corresponding antiparticle. This is mathematically contained in the spinor fields which are the solutions of the relativistic wave equations.

Charge conjugation switches particles and antiparticles. Physical laws and interactions unchanged by this operation have C symmetry.

- Parity mirrors the orientation of the spatial coordinates from left-handed to right-handed. Informally, space is "reflected" into its mirror image. Physical laws and interactions unchanged by this operation have P symmetry.
- Time reversal flips the time coordinate, which amounts to time running from future to past. A curious property of time, which space does not have, is that it is unidirectional: particles traveling forwards in time are equivalent to antiparticles traveling back in time. Physical laws and interactions unchanged by this operation have T symmetry.

In quantum electrodynamics, the symmetry group is U(1) and is abelian. In quantum chromodynamics, the symmetry group is SU(3) and is non-abelian.

The electromagnetic interaction is mediated by photons, which have no electric charge. The electromagnetic tensor has an electromagnetic four-potential field possessing gauge symmetry.

The strong (color) interaction is mediated by gluons, which can have eight color charges. There are eight gluon field strength tensors with corresponding gluon four potentials field, each possessing gauge symmetry.

Analogous to the spin operator, there are color charge operators in terms of the Gell-Mann matrices *λ _{j}*:

and since color charge is a conserved charge, all color charge operators must commute with the Hamiltonian:

Isospin is conserved in strong interactions.

Magnetic monopoles can be theoretically realized, although current observations and theory are consistent with them existing or not existing. Electric and magnetic charges can effectively be "rotated into one another" by a duality transformation.

A Lie superalgebra is an algebra in which (suitable) basis elements either have a commutation relation or have an anticommutation relation. Symmetries have been proposed to the effect that all fermionic particles have bosonic analogues, and vice versa. These symmetry have theoretical appeal in that no extra assumptions (such as existence of strings) barring symmetries are made. In addition, by assuming supersymmetry, a number of puzzling issues can be resolved. These symmetries, which are represented by Lie superalgebras, have not been confirmed experimentally. It is now believed that they are broken symmetries, if they exist. But it has been speculated that dark matter is constitutes gravitinos, a spin 3/2 particle with mass, its supersymmetric partner being the graviton.

The concept of **exchange symmetry** or **permutation symmetry** is derived from a fundamental postulate of quantum statistics, which states that no observable physical quantity should change after exchanging two identical particles. It states that because all observables are proportional to for a system of identical particles, the wave function must either remain the same or change sign upon such an exchange. More generally, for a system of *n* identical particles the wave function must transform as an irreducible representation of the finite symmetric group **S _{n}**. It turns out that, according to the Spin-statistics theorem, fermion states transform as the antisymmetric irreducible representation of

Because the exchange of two identical particles is mathematically equivalent to the rotation of each particle by 180 degrees (and so to the rotation of one particle's frame by 360 degrees),^{ [15] } the symmetric nature of the wave function depends on the particle's spin after the rotation operator is applied to it. Integer spin particles do not change the sign of their wave function upon a 360 degree rotation—therefore the sign of the wave function of the entire system does not change. Semi-integer spin particles change the sign of their wave function upon a 360 degree rotation (see more in spin–statistics theorem).

Particles for which the wave function does not change sign upon exchange are called bosons, or particles with a symmetric wave function. The particles for which the wave function of the system changes sign are called fermions, or particles with an antisymmetric wave function.

Fermions therefore obey different statistics (called Fermi–Dirac statistics) than bosons (which obey Bose–Einstein statistics). One of the consequences of Fermi–Dirac statistics is the exclusion principle for fermions—no two identical fermions can share the same quantum state (in other words, the wave function of two identical fermions in the same state is zero). This in turn results in degeneracy pressure for fermions—the strong resistance of fermions to compression into smaller volume. This resistance gives rise to the “stiffness” or “rigidity” of ordinary atomic matter (as atoms contain electrons which are fermions).

- Symmetric group
- Spin-statistics theorem
- Projective representation
- Casimir operator
- Pauli–Lubanski pseudovector
- Symmetries in general relativity
- Renormalization group
- Center of mass (relativistic)
- Representation of a Lie group
- Representation theory of the Poincaré group
- Representation theory of the Lorentz group

In physics, the **Lorentz transformations** are a one-parameter family of linear transformations from a coordinate frame in spacetime to another frame that moves at a constant velocity relative to the former. The respective inverse transformation is then parametrized by the negative of this velocity. The transformations are named after the Dutch physicist Hendrik Lorentz.

In mathematical physics and mathematics, the **Pauli matrices** are a set of three 2 × 2 complex matrices which are Hermitian and unitary. Usually indicated by the Greek letter sigma, they are occasionally denoted by tau when used in connection with isospin symmetries. They are

The **Schrödinger equation** is a linear partial differential equation that describes the wave function or state function of a quantum-mechanical system. It is a key result in quantum mechanics, and its discovery was a significant landmark in the development of the subject. The equation is named after Erwin Schrödinger, who postulated the equation in 1925, and published it in 1926, forming the basis for the work that resulted in his Nobel Prize in Physics in 1933.

A **wave function** in quantum physics is a mathematical description of the quantum state of an isolated quantum system. The wave function is a complex-valued probability amplitude, and the probabilities for the possible results of measurements made on the system can be derived from it. The most common symbols for a wave function are the Greek letters *ψ* and Ψ.

In mechanics and geometry, the **3D rotation group**, often denoted **SO(3)**, is the group of all rotations about the origin of three-dimensional Euclidean space under the operation of composition. By definition, a rotation about the origin is a transformation that preserves the origin, Euclidean distance, and orientation. Every non-trivial rotation is determined by its axis of rotation and its angle of rotation. Composing two rotations results in another rotation; every rotation has a unique inverse rotation; and the identity map satisfies the definition of a rotation. Owing to the above properties, the set of all rotations is a group under composition. Rotations are not commutative, making it a nonabelian group. Moreover, the rotation group has a natural structure as a manifold for which the group operations are smoothly differentiable; so it is in fact a Lie group. It is compact and has dimension 3.

In special relativity, a **four-vector** is an object with four components, which transform in a specific way under Lorentz transformation. Specifically, a four-vector is an element of a four-dimensional vector space considered as a representation space of the standard representation of the Lorentz group, the (½,½) representation. It differs from a Euclidean vector in how its magnitude is determined. The transformations that preserve this magnitude are the Lorentz transformations, which include spatial rotations and boosts.

In physics, an **operator** is a function over a space of physical states onto another space of physical states. The simplest example of the utility of operators is the study of symmetry. Because of this, they are very useful tools in classical mechanics. Operators are even more important in quantum mechanics, where they form an intrinsic part of the formulation of the theory.

In physics, specifically relativistic quantum mechanics (RQM) and its applications to particle physics, **relativistic wave equations** predict the behavior of particles at high energies and velocities comparable to the speed of light. In the context of quantum field theory (QFT), the equations determine the dynamics of quantum fields.

In quantum mechanics and computing, the **Bloch sphere** is a geometrical representation of the pure state space of a two-level quantum mechanical system (qubit), named after the physicist Felix Bloch.

In quantum mechanics, a **parity transformation** is the flip in the sign of *one* spatial coordinate. In three dimensions, it can also refer to the simultaneous flip in the sign of all three spatial coordinates :

In quantum mechanics, a **two-state system** is a quantum system that can exist in any quantum superposition of two independent quantum states. The Hilbert space describing such a system is two-dimensional. Therefore, a complete basis spanning the space will consist of two independent states. Any two-state system can also be seen as a qubit.

This article describes the mathematics of the **Standard Model** of particle physics, a gauge quantum field theory containing the internal symmetries of the unitary product group SU(3) × SU(2) × U(1). The theory is commonly viewed as containing the fundamental set of particles – the leptons, quarks, gauge bosons and the Higgs particle.

In quantum mechanics, the **angular momentum operator** is one of several related operators analogous to classical angular momentum. The angular momentum operator plays a central role in the theory of atomic and molecular physics and other quantum problems involving rotational symmetry. In both classical and quantum mechanical systems, angular momentum is one of the three fundamental properties of motion.

**Photon polarization** is the quantum mechanical description of the classical polarized sinusoidal plane electromagnetic wave. An individual photon can be described as having right or left circular polarization, or a superposition of the two. Equivalently, a photon can be described as having horizontal or vertical linear polarization, or a superposition of the two.

In physics, **relativistic quantum mechanics (RQM)** is any Poincaré covariant formulation of quantum mechanics (QM). This theory is applicable to massive particles propagating at all velocities up to those comparable to the speed of light *c*, and can accommodate massless particles. The theory has application in high energy physics, particle physics and accelerator physics, as well as atomic physics, chemistry and condensed matter physics. *Non-relativistic quantum mechanics* refers to the mathematical formulation of quantum mechanics applied in the context of Galilean relativity, more specifically quantizing the equations of classical mechanics by replacing dynamical variables by operators. *Relativistic quantum mechanics* (RQM) is quantum mechanics applied with special relativity. Although the earlier formulations, like the Schrödinger picture and Heisenberg picture were originally formulated in a non-relativistic background, a few of them also work with special relativity.

In quantum mechanics and particle physics, **spin** is an intrinsic form of angular momentum carried by elementary particles, composite particles (hadrons), and atomic nuclei.

In theoretical physics, the composition of two non-collinear Lorentz boosts results in a Lorentz transformation that is not a pure boost but is the composition of a boost and a rotation. This rotation is called **Thomas rotation**, **Thomas–Wigner rotation** or **Wigner rotation**. The rotation was discovered by Llewellyn Thomas in 1926, and derived by Wigner in 1939. If a sequence of non-collinear boosts returns an object to its initial velocity, then the sequence of Wigner rotations can combine to produce a net rotation called the Thomas precession.

In relativistic quantum mechanics and quantum field theory, the **Bargmann–Wigner equations** describe free particles of arbitrary spin *j*, an integer for bosons or half-integer for fermions. The solutions to the equations are wavefunctions, mathematically in the form of multi-component spinor fields.

In pure and applied mathematics, quantum mechanics and computer graphics, a **tensor operator** generalizes the notion of operators which are scalars and vectors. A special class of these are **spherical tensor operators** which apply the notion of the spherical basis and spherical harmonics. The spherical basis closely relates to the description of angular momentum in quantum mechanics and spherical harmonic functions. The coordinate-free generalization of a tensor operator is known as a **representation operator**.

Attempts have been made to describe gauge theories in terms of extended objects such as Wilson loops and holonomies. The **loop representation** is a quantum hamiltonian representation of gauge theories in terms of loops. The aim of the loop representation in the context of Yang–Mills theories is to avoid the redundancy introduced by Gauss gauge symmetries allowing to work directly in the space of physical states. The idea is well known in the context of lattice Yang–Mills theory. Attempts to explore the continuous loop representation was made by Gambini and Trias for canonical Yang–Mills theory, however there were difficulties as they represented singular objects. As we shall see the loop formalism goes far beyond a simple gauge invariant description, in fact it is the natural geometrical framework to treat gauge theories and quantum gravity in terms of their fundamental physical excitations.

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*Lie Groups, Lie Algebras, and Representations: An Elementary Introduction*. Graduate Texts in Mathematics.**222**(2nd ed.). Springer. - ↑ Hall, Brian C. (2013).
*Quantum Theory for Mathematicians*. Graduate Texts in Mathematics. Springer. - ↑ C.B. Parker (1994).
*McGraw Hill Encyclopaedia of Physics*(2nd ed.). McGraw Hill. p. 1333. ISBN 0-07-051400-3. - ↑ T. Ohlsson (2011).
*Relativistic Quantum Physics: From Advanced Quantum Mechanics to Introductory Quantum Field Theory*. Cambridge University Press. pp. 7–10. ISBN 978-1-13950-4324. - ↑ E. Abers (2004).
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*Lorentz Transformations*. arXiv: 1103.0156 . - ↑ H.L. Berk; K. Chaicherdsakul; T. Udagawa. "The Proper Homogeneous Lorentz Transformation Operator
*e*=^{L}*e*^{− ω·S − ξ·K}, Where's It Going, What's the Twist" (PDF). Texas, Austin. - ↑ Weinberg, S. (1964). "Feynman Rules
*for Any*spin" (PDF).*Phys. Rev*.**133**(5B): B1318–B1332. Bibcode:1964PhRv..133.1318W. doi:10.1103/PhysRev.133.B1318.; Weinberg, S. (1964). "Feynman Rules*for Any*spin. II. Massless Particles" (PDF).*Phys. Rev*.**134**(4B): B882–B896. Bibcode:1964PhRv..134..882W. doi:10.1103/PhysRev.134.B882.; Weinberg, S. (1969). "Feynman Rules*for Any*spin. III" (PDF).*Phys. Rev*.**181**(5): 1893–1899. Bibcode:1969PhRv..181.1893W. doi:10.1103/PhysRev.181.1893. - ↑ K. Masakatsu (2012). "Superradiance Problem of Bosons and Fermions for Rotating Black Holes in Bargmann–Wigner Formulation". Nara, Japan. arXiv: 1208.0644 .Cite journal requires
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(help) - ↑ N.N. Bogolubov (1989).
*General Principles of Quantum Field Theory*(2nd ed.). Springer. p. 272. ISBN 0-7923-0540-X. - ↑ T. Ohlsson (2011).
*Relativistic Quantum Physics: From Advanced Quantum Mechanics to Introductory Quantum Field Theory*. Cambridge University Press. p. 10. ISBN 978-1-13950-4324. - ↑ D. Bonastos; et al. (1994). "Symmetry Algebra of the Planar Anisotropic Quantum Harmonic Oscillator with Rational Ratio of Frequencies". arXiv: hep-th/9402099 .
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*Lie Groups, Lie Algebras, and Representations: An Elementary Introduction*. Graduate Texts in Mathematics.**222**(2nd ed.). Springer. Chapter 6 - ↑ Longuet-Higgins, H.C. (1963). "The symmetry groups of non-rigid molecules".
*Molecular Physics*.**6**(5): 445–460. Bibcode:1963MolPh...6..445L. doi: 10.1080/00268976300100501 . - ↑ Feynman, Richard (13 July 1999).
*The 1986 Dirac Memorial Lectures*. Cambridge University Press. p. 57. ISBN 978-0-521-65862-1.

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*Symmetries and Conservation Laws in Particle Physics: An Introduction to Group Theory for Particle Physicists*. World Scientific. ISBN 978-184-816-703-2. - M. F. C. Ladd (1989).
*Symmetry in molecules and crystals*. Solid state science. Ellis Horwood series in physical chemistry. ISBN 0-85312-255-5. - W. Ludwig; C. Falter (1996).
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*A Derivation of the Quantum Mechanical Momentum Operator in the Position Representation* - D. E. Soper (2011)
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