# Angular momentum operator

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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 physics and other quantum problems involving rotational symmetry. In both classical and quantum mechanical systems, angular momentum (together with linear momentum and energy) is one of the three fundamental properties of motion.

There are several angular momentum operators: total angular momentum (usually denoted J), orbital angular momentum (usually denoted L), and spin angular momentum (spin for short, usually denoted S). The term "angular momentum operator" can (confusingly) refer to either the total or the orbital angular momentum. Total angular momentum is always conserved, see Noether's theorem.

## Spin, orbital, and total angular momentum

{{#invoke:main|main}} "Vector cones" of total angular momentum J (purple), orbital L (blue), and spin S (green). The cones arise due to quantum uncertainty between measuring angular momentum components (see below).

The classical definition of angular momentum is $\mathbf {L} =\mathbf {r} \times \mathbf {p}$ . This can be carried over to quantum mechanics, by reinterpreting r as the quantum position operator and p as the quantum momentum operator. L is then an operator, specifically called the orbital angular momentum operator. Specifically, L is a vector operator, meaning ${\mathbf {L} }=(L_{x},L_{y},L_{z})$ , where Lx, Ly, Lz are three different operators.

However, there is another type of angular momentum, called spin angular momentum (more often shortened to spin), represented by the spin operator S. Almost all elementary particles have spin. Spin is often depicted as a particle literally spinning around an axis, but this is a misleading and inaccurate picture: Spin is an intrinsic property of a particle, unrelated to any sort of motion in space. All elementary particles have a characteristic spin, for example electrons always have "spin 1/2" while photons always have "spin 1".

Finally, there is total angular momentum J, which combines both the spin and orbital angular momentum of a particle or system:

${\mathbf {J} }={\mathbf {L} }+{\mathbf {S} }.$ Conservation of angular momentum states that J for a closed system, or J for the whole universe, is conserved. However, L and S are not generally conserved. For example, the spin–orbit interaction allows angular momentum to transfer back and forth between L and S, with the total J remaining constant.

## Orbital angular momentum operator

The orbital angular momentum operator L is mathematically defined as the cross product of a wave function's position operator (r) and momentum operator (p):

$\mathbf {L} =\mathbf {r} \times \mathbf {p}$ This is analogous to the definition of angular momentum in classical physics.

In the special case of a single particle with no electric charge and no spin, the angular momentum operator can be written in the position basis as a single vector equation:

${\mathbf {L} }=-i\hbar ({\mathbf {r} }\times \nabla )$ where ∇ is the vector differential operator, del.

## Commutation relations

### Commutation relations between components

The orbital angular momentum operator is a vector operator, meaning it can be written in terms of its vector components ${\mathbf {L} }=(L_{x},L_{y},L_{z})$ . The components have the following commutation relations with each other:

$[L_{x},L_{y}]=i\hbar L_{z},\;\;[L_{y},L_{z}]=i\hbar L_{x},\;\;[L_{z},L_{x}]=i\hbar L_{y},$ where [ , ] denotes the commutator

$[X,Y]\equiv XY-YX.$ This can be written generally as

$[L_{l},L_{m}]=i\hbar \sum _{n=1}^{3}\varepsilon _{lmn}L_{n}$ ,

where l, m, n are the component indices (1 for x, 2 for y, 3 for z), and εlmn denotes the Levi-Civita symbol.

A compact expression as one vector equation is also possible:

$\mathbf {L} \times \mathbf {L} =i\hbar \mathbf {L}$ The commutation relations can be proved as a direct consequence of the canonical commutation relations $[x_{l},p_{m}]=i\hbar \delta _{lm}$ , where δlm is the Kronecker delta.

The same commutation relations apply for the other angular momentum operators (spin and total angular momentum):

$[S_{l},S_{m}]=i\hbar \sum _{n=1}^{3}\varepsilon _{lmn}S_{n},\quad [J_{l},J_{m}]=i\hbar \sum _{n=1}^{3}\varepsilon _{lmn}J_{n}$ .

These can be assumed to hold in analogy with L. Alternatively, they can be derived as discussed below.

These commutation relations mean that L has the mathematical structure of a Lie algebra. In this case, the Lie algebra is SU(2) or SO(3), the rotation group in three dimensions. The same is true of J and S. The reason is discussed below. These commutation relations are relevant for measurement and uncertainty, as discussed further below.

#### Analogy to Poisson brackets in classical physics

There is an analogous relationship to the commutator in classical physics which is central to the theory of canonical transformations of Hamilton's equations of motion:

$[u,v]_{q,p}={\frac {\partial u}{\partial q_{i}}}{\frac {\partial v}{\partial p_{i}}}-{\frac {\partial u}{\partial p_{i}}}{\frac {\partial v}{\partial q_{i}}}\!$ (summation over generalized coordinate index i implied) where, in this bilinear expression, $[u,v]_{q,p}$ is the Poisson bracket of two functions $u,v$ with respect to the canonical (generalized) coordinates $(p,q)$ . "... identification of the canonical angular momentum as the generator of rigid rotation of [a system of particles] leads to a number of interesting and important Poisson bracket relations." Among these are:

$[L_{l},L_{m}]=\varepsilon _{lmn}L_{n}.\!$ Here, $L_{z}$ , for example, is a transformation generated by the generalized momentum conjugate to $q_{i}$ :

$L_{z}(q,p)=p_{i}$ .

It can be shown (using Cartesian coordinates x, y and z for each particle i in the system) that

$L_{z}=x_{i}p_{iy}-y_{i}p_{ix}$ .

This generating function $L_{z}$ has the physical significance of being the z-component of the total angular momentum:

$L_{z}\ \equiv \ (r_{i}\ \times \ p_{i})_{z}$ .

It is important to recognize that the Poisson bracket is an analogue, not the commutator in disguise. Hamilton's equations do not generalize to quantum mechanics because they assume that the position and momentum of a particle can be known simultaneously to infinite precision at any point in time. See the section "Generalization to quantum mechanics through Poisson bracket" in the article on Hamiltonian mechanics for details and additional references.

### Commutation relations involving vector magnitude

Like any vector, a magnitude can be defined for the orbital angular momentum operator,

$L^{2}\equiv L_{x}^{2}+L_{y}^{2}+L_{z}^{2}$ .

L2 is another quantum operator. It commutes with the components of L,

$[L^{2},L_{x}]=[L^{2},L_{y}]=[L^{2},L_{z}]=0~.\,$ One way to prove that these operators commute is to start from the [L, Lm] commutation relations in the previous section:

Mathematically, L2 is a Casimir invariant of the Lie algebra so(3) spanned by L.

In the classical case, L is the orbital angular momentum of the entire system of particles, n is the unit vector along one of the Cartesian axes, and we also have Poisson bracket pseudo-commutation of L with each of its Cartesian components:

$[\mathbf {L} \cdot \mathbf {L} ,\mathbf {L} \cdot \mathbf {n} ]=[L^{2},\mathbf {L} \cdot \mathbf {n} ]=0~,$ with n selecting one of the three Cartesian components of L.

The same commutation relations apply to the other angular momentum operators (spin and total angular momentum), as well,

{\begin{aligned}{[}S^{2},S_{i}]&=0,\\{[}J^{2},J_{i}]&=0.\end{aligned}} ### Uncertainty principle

{{#invoke:main|main}} In general, in quantum mechanics, when two observable operators do not commute, they are called incompatible observables. Two incompatible observables cannot be measured simultaneously; instead they satisfy an uncertainty principle. The more accurately one observable is known, the less accurately the other one can be known. Just as there is an uncertainty principle relating position and momentum, there are uncertainty principles for angular momentum.

The Robertson–Schrödinger relation gives the following uncertainty principle:

$\sigma _{L_{x}}\sigma _{L_{y}}\geq {\frac {\hbar }{2}}\left|\langle L_{z}\rangle \right|.$ where $\sigma _{X}$ is the standard deviation in the measured values of X and $\langle X\rangle$ denotes the expectation value of X. This inequality is also true if x,y,z are rearranged, or if L is replaced by J or S.

Therefore, two orthogonal components of angular momentum cannot be simultaneously known or measured, except in special cases such as $L_{x}=L_{y}=L_{z}=0$ .

It is, however, possible to simultaneously measure or specify L2 and any one component of L; for example, L2 and Lz. This is often useful, and the values are characterized by azimuthal quantum number and magnetic quantum number, as discussed further below.

## Quantization

{{#invoke:see also|seealso}} In quantum mechanics, angular momentum is quantized – that is, it cannot vary continuously, but only in "quantum leaps" between certain allowed values. For any system, the following restrictions on measurement results apply, where $\hbar$ is reduced Planck constant: In this standing wave on a circular string, the circle is broken into exactly 8 wavelengths. A standing wave like this can have 0,1,2, or any integer number of wavelengths around the circle, but it cannot have a non-integer number of wavelengths like 8.3. In quantum mechanics, angular momentum is quantized for a similar reason.

{{#invoke:main|main}} A common way to derive the quantization rules above is the method of ladder operators. The ladder operators are defined:

{\begin{aligned}J_{+}&\equiv J_{x}+iJ_{y},\\J_{-}&\equiv J_{x}-iJ_{y}\end{aligned}} By manipulating these ladder operators and using the commutation rules, it is possible to prove almost all of the quantization rules above.

Since S and L have the same commutation relations as J, the same ladder analysis works for them.

The ladder-operator analysis does not explain one aspect of the quantization rules above: the fact that L (unlike J and S) cannot have half-integer quantum numbers. This fact can be proven (at least in the special case of one particle) by writing down every possible eigenfunction of L2 and Lz, (they are the spherical harmonics), and seeing explicitly that none of them have half-integer quantum numbers. An alternative derivation is below.

### Visual interpretation

{{#invoke:main|main}} Since the angular momenta are quantum operators, they cannot be drawn as vectors like in classical mechanics. Nevertheless, it is common to depict them heuristically in this way. Depicted on the right is a set of states with quantum numbers $\ell =2$ , and $m_{\ell }=-2,-1,0,1,2$ for the five cones from bottom to top. Since $|L|={\sqrt {L^{2}}}=\hbar {\sqrt {6}}$ , the vectors are all shown with length $\hbar {\sqrt {6}}$ . The rings represent the fact that $L_{z}$ is known with certainty, but $L_{x}$ and $L_{y}$ are unknown; therefore every classical vector with the appropriate length and z-component is drawn, forming a cone. The expected value of the angular momentum for a given ensemble of systems in the quantum state characterized by $\ell$ and $m_{\ell }$ could be somewhere on this cone while it cannot be defined for a single system (since the components of $L$ do not commute with each other).

### Quantization in macroscopic systems

The quantization rules are technically true even for macroscopic systems, like the angular momentum L of a spinning tire. However they have no observable effect. For example, if $L_{z}/\hbar$ is roughly 100000000, it makes essentially no difference whether the precise value is an integer like 100000000 or 100000001, or a non-integer like 100000000.2—the discrete steps are too small to notice.

## Angular momentum as the generator of rotations

{{#invoke:see also|seealso}} The most general and fundamental definition of angular momentum is as the generator of rotations. More specifically, let $R({\hat {n}},\phi )$ be a rotation operator, which rotates any quantum state about axis ${\hat {n}}$ by angle $\phi$ . As $\phi \rightarrow 0$ , the operator $R({\hat {n}},\phi )$ approaches the identity operator, because a rotation of 0° maps all states to themselves. Then the angular momentum operator $J_{\hat {n}}$ about axis ${\hat {n}}$ is defined as:

$J_{\hat {n}}\equiv i\hbar \lim _{\phi \rightarrow 0}{\frac {R({\hat {n}},\phi )-1}{\phi }}$ where 1 is the identity operator. Remark also that R is an additive morphism : $R({\hat {n}},\phi _{1}+\phi _{2})=R({\hat {n}},\phi _{1})R({\hat {n}},\phi _{2})$ ; as a consequence

$R({\hat {n}},\phi )=\exp(-i\phi J_{\hat {n}}/\hbar )$ where exp is matrix exponential.

In simpler terms, the total angular momentum operator characterizes how a quantum system is changed when it is rotated. The relationship between angular momentum operators and rotation operators is the same as the relationship between Lie algebras and Lie groups in mathematics, as discussed further below. The different types of rotation operators. Top: Two particles, with spin states indicated schematically by the arrows. (A) The operator R, related to J, rotates the entire system. (B) The operator Rspatial, related to L, rotates the particle positions without altering their internal spin states. (C) The operator Rinternal, related to S, rotates the particles' internal spin states without changing their positions.

Just as J is the generator for rotation operators, L and S are generators for modified partial rotation operators. The operator

$R_{\mathrm {spatial} }({\hat {n}},\phi )=\exp(-i\phi L_{\hat {n}}/\hbar ),$ rotates the position (in space) of all particles and fields, without rotating the internal (spin) state of any particle. Likewise, the operator

$R_{\mathrm {internal} }({\hat {n}},\phi )=\exp(-i\phi S_{\hat {n}}/\hbar ),$ rotates the internal (spin) state of all particles, without moving any particles or fields in space. The relation J=L+S comes from:

$R({\hat {n}},\phi )=R_{\mathrm {internal} }({\hat {n}},\phi )R_{\mathrm {spatial} }({\hat {n}},\phi )$ i.e. if the positions are rotated, and then the internal states are rotated, then altogether the complete system has been rotated.

### SU(2), SO(3), and 360° rotations

{{#invoke:main|main}} Although one might expect $R({\hat {n}},360^{\circ })=1$ (a rotation of 360° is the identity operator), this is not assumed in quantum mechanics, and it turns out it is often not true: When the total angular momentum quantum number is a half-integer (1/2, 3/2, etc.), $R({\hat {n}},360^{\circ })=-1$ , and when it is an integer, $R({\hat {n}},360^{\circ })=+1$ . Mathematically, the structure of rotations in the universe is not SO(3), the group of three-dimensional rotations in classical mechanics. Instead, it is SU(2), which is identical to SO(3) for small rotations, but where a 360° rotation is mathematically distinguished from a rotation of 0°. (A rotation of 720° is, however, the same as a rotation of 0°.)

On the other hand, $R_{\mathrm {spatial} }({\hat {n}},360^{\circ })=+1$ in all circumstances, because a 360° rotation of a spatial configuration is the same as no rotation at all. (This is different from a 360° rotation of the internal (spin) state of the particle, which might or might not be the same as no rotation at all.) In other words, the $R_{\mathrm {spatial} }$ operators carry the structure of SO(3), while $R$ and $R_{\mathrm {internal} }$ carry the structure of SU(2).

$e^{-2\pi im}=1$ which is to say that the orbital angular momentum quantum numbers can only be integers, not half-integers.

### Connection to representation theory

{{#invoke:main|main}} Starting with a certain quantum state $|\psi _{0}\rangle$ , consider the set of states $R({\hat {n}},\phi )|\psi _{0}\rangle$ for all possible ${\hat {n}}$ and $\phi$ , i.e. the set of states that come about from rotating the starting state in every possible way. This is a vector space, and therefore the manner in which the rotation operators map one state onto another is a representation of the group of rotation operators.

When rotation operators act on quantum states, it forms a representation of the Lie group SU(2) (for R and Rinternal), or SO(3) (for Rspatial).

From the relation between J and rotation operators,

When angular momentum operators act on quantum states, it forms a representation of the Lie algebra SU(2) or SO(3).

(The Lie algebras of SU(2) and SO(3) are identical.)

The ladder operator derivation above is a method for classifying the representations of the Lie algebra SU(2).

### Connection to commutation relations

Classical rotations do not commute with each other: For example, rotating 1° about the x-axis then 1° about the y-axis gives a slightly different overall rotation than rotating 1° about the y-axis then 1° about the x-axis. By carefully analyzing this noncommutativity, the commutation relations of the angular momentum operators can be derived.

(This same calculational procedure is one way to answer the mathematical question "What is the Lie algebra of the Lie groups SO(3) or SU(2)?")

## Conservation of angular momentum

The Hamiltonian H represents the energy and dynamics of the system. In a spherically-symmetric situation, the Hamiltonian is invariant under rotations:

$RHR^{-1}=H$ where R is a rotation operator. As a consequence, $[H,R]=0$ , and then $[H,\mathbf {J} ]=\mathbf {0}$ due to the relationship between J and R. By the Ehrenfest theorem, it follows that J is conserved.

To summarize, if H is rotationally-invariant (spherically symmetric), then total angular momentum J is conserved. This is an example of Noether's theorem.

If H is just the Hamiltonian for one particle, the total angular momentum of that one particle is conserved when the particle is in a central potential (i.e., when the potential energy function depends only on $|{\mathbf {r} }|$ ). Alternatively, H may be the Hamiltonian of all particles and fields in the universe, and then H is always rotationally-invariant, as the fundamental laws of physics of the universe are the same regardless of orientation. This is the basis for saying conservation of angular momentum is a general principle of physics.

For a particle without spin, J=L, so orbital angular momentum is conserved in the same circumstances. When the spin is nonzero, the spin-orbit interaction allows angular momentum to transfer from L to S or back. Therefore, L is not, on its own, conserved.

## Angular momentum coupling

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Often, two or more sorts of angular momentum interact with each other, so that angular momentum can transfer from one to the other. For example, in spin-orbit coupling, angular momentum can transfer between L and S, but only the total J=L+S is conserved. In another example, in an atom with two electrons, each has its own angular momentum J1 and J2, but only the total J=J1+J2 is conserved.

In these situations, it is often useful to know the relationship between, on the one hand, states where $(J_{1})_{z},(J_{1})^{2},(J_{2})_{z},(J_{2})^{2}$ all have definite values, and on the other hand, states where $(J_{1})^{2},(J_{2})^{2},J^{2},J_{z}$ all have definite values, as the latter four are usually conserved (constants of motion). The procedure to go back and forth between these bases is to use Clebsch–Gordan coefficients.

One important result in this field is that a relationship between the quantum numbers for $(J_{1})^{2},(J_{2})^{2},J^{2}$ :

$j\in \{|j_{1}-j_{2}|,(|j_{1}-j_{2}|+1),\ldots ,(j_{1}+j_{2})\}$ .

For an atom or molecule with J = L + S, the term symbol gives the quantum numbers associated with the operators $L^{2},S^{2},J^{2}$ .

## Orbital angular momentum in spherical coordinates

Angular momentum operators usually occur when solving a problem with spherical symmetry in spherical coordinates. The angular momentum in space representation is 

{\begin{aligned}L_{x}&=i\hbar \left(\sin \phi {\frac {\partial }{\partial \theta }}+\cot \theta \cos \phi {\frac {\partial }{\partial \phi }}\right),\\L_{y}&=i\hbar \left(-\cos \phi {\frac {\partial }{\partial \theta }}+\cot \theta \sin \phi {\frac {\partial }{\partial \phi }}\right),\\L_{z}&=-i\hbar {\frac {\partial }{\partial \phi ,}}\end{aligned}} and

{\begin{aligned}L_{+}&=\hbar e^{i\phi }\left({\frac {\partial }{\partial \theta }}+i\cot \theta {\frac {\partial }{\partial \phi }}\right),\\L_{-}&=\hbar e^{-i\phi }\left(-{\frac {\partial }{\partial \theta }}+i\cot \theta {\frac {\partial }{\partial \phi }}\right),\\L^{2}&=-\hbar ^{2}\left({\frac {1}{\sin \theta }}{\frac {\partial }{\partial \theta }}\left[\sin \theta {\frac {\partial }{\partial \theta }}\right]+{\frac {1}{\sin ^{2}\theta }}{\frac {\partial ^{2}}{\partial \phi ^{2}}}\right).\end{aligned}} When solving to find eigenstates of this operator, we obtain the following

{\begin{aligned}L^{2}\mid l,m\rangle &={\hbar }^{2}l(l+1)|l,m\rangle \\L_{z}\mid l,m\rangle &=\hbar m|l,m\rangle \end{aligned}} where

$\langle \theta ,\phi |l,m\rangle =Y_{l,m}(\theta ,\phi )$ are the spherical harmonics.