Angular momentum (quantum)

In quantum mechanics, angular momentum is a vector operator of which the three components have well-defined commutation relations. This operator is the quantum analogue of the classical angular momentum vector.

Angular momentum entered quantum mechanics in one of the very first—and most important—papers on the "new" quantum mechanics, the Dreimännerarbeit (three men's work) of Born, Heisenberg and Jordan (1926). In this paper the orbital angular momentum and its eigenstates are already fully covered by the algebraic techniques of commutation relations and step up/down operators that will be treated in the present article. In 1927, Wolfgang Pauli introduced spin angular momentum, which is a form of angular momentum without a classical counterpart.

Angular momentum theory—together with its connection to group theory— brought order to a bewildering number of spectroscopic observations in atomic spectroscopy, see, for instance, Wigner's seminal work. When in 1926 electron spin was discovered and Pauli proved less than a year later that spin was a form of angular momentum, its importance rose even further. To date the theory of angular momentum is of great importance in quantum mechanics. It is an indispensable discipline for the working physicist, irrespective of his field of specialization, be it solid state physics, molecular-, atomic,- nuclear,- or even hadronic-structure physics.

Orbital angular momentum

The classical angular momentum of a point mass is,

$\mathbf {L} =\mathbf {r} \times \mathbf {p} ,$

where r is the position and p the (linear) momentum of the point mass. The simplest and oldest example of an angular momentum operator is obtained by applying the quantization rule:

$\mathbf {p} \rightarrow -i\hbar \mathbf {\nabla } ,$

where $\scriptstyle \hbar$ is Planck's constant (divided by 2π) and ∇ is the gradient operator. This rule applied to the classical angular momentum vector gives a vector operator with the following three components,

${\begin{aligned}L_{x}&=-i\hbar {\Big (}y{\frac {\partial }{\partial z}}-z{\frac {\partial }{\partial y}}{\Big )}\\L_{y}&=-i\hbar {\Big (}z{\frac {\partial }{\partial x}}-x{\frac {\partial }{\partial z}}{\Big )}\\L_{z}&=-i\hbar {\Big (}x{\frac {\partial }{\partial y}}-y{\frac {\partial }{\partial x}}{\Big )}.\\\end{aligned}}$

The following commutation relations can be proved,

$[L_{x},\,L_{y}]=i\hbar L_{z},\quad [L_{z},\,L_{x}]=i\hbar L_{y},\quad [L_{y},\,L_{z}]=i\hbar L_{x}.$

The square brackets indicate the commutator of two operators, defined for two arbitrary operators A and B as

$[A,\,B]\equiv AB-BA.$

For instance,

${\begin{aligned}{\big [}L_{x},\,L_{y}{\big ]}=&-\hbar ^{2}\left[{\Big (}y{\frac {\partial }{\partial z}}-z{\frac {\partial }{\partial y}}{\Big )}{\Big (}z{\frac {\partial }{\partial x}}-x{\frac {\partial }{\partial z}}{\Big )}-{\Big (}z{\frac {\partial }{\partial x}}-x{\frac {\partial }{\partial z}}{\Big )}{\Big (}y{\frac {\partial }{\partial z}}-z{\frac {\partial }{\partial y}}{\Big )}\right]\\=&-\hbar ^{2}\left[y{\frac {\partial }{\partial x}}-x{\frac {\partial }{\partial y}}\right]=i\hbar \left[-i\hbar {\Big (}x{\frac {\partial }{\partial y}}-y{\frac {\partial }{\partial x}}{\Big )}\right]=i\hbar L_{z},\\\end{aligned}}$

where we used that all the terms of the kind

$yx{\frac {\partial ^{2}}{\partial z\partial x}},\quad {\hbox{etc.}}$

mutually cancel.

The total angular momentum squared is defined by

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

In terms of spherical polar coordinates the operator is,

$L^{2}=-\left[{\frac {1}{\sin \theta }}{\frac {\partial }{\partial \theta }}\sin \theta {\frac {\partial }{\partial \theta }}+{\frac {1}{\sin ^{2}\theta }}{\frac {\partial ^{2}}{\partial \varphi ^{2}}}\right].$

Note, parenthetically, that eigenfunctions of the latter operator have been known since the nineteenth century, long before quantum mechanics was born. They are spherical harmonic functions.

Spin angular momentum

Pauli introduced in 1927 the following three matrices, which are now known as Pauli spin matrices,

${\boldsymbol {\sigma }}_{x}={\begin{pmatrix}0&1\\1&0\\\end{pmatrix}},\qquad {\boldsymbol {\sigma }}_{y}={\begin{pmatrix}0&-i\\i&0\\\end{pmatrix}},\qquad {\boldsymbol {\sigma }}_{z}={\begin{pmatrix}1&0\\0&-1\\\end{pmatrix}}.$

These Hermitian matrices represent Hermitian operators on a two-dimensional linear space over the field of complex numbers: spin space. Spin angular momentum operators are defined by

$s_{x}\leftrightarrow {\frac {\hbar }{2}}{\boldsymbol {\sigma }}_{x}\qquad s_{y}\leftrightarrow {\frac {\hbar }{2}}{\boldsymbol {\sigma }}_{y}\qquad s_{z}\leftrightarrow {\frac {\hbar }{2}}{\boldsymbol {\sigma }}_{z}.$

The commutation relations of these operators follow by matrix multiplication, for instance,

$[s_{x},\,s_{y}]\leftrightarrow {\frac {\hbar ^{2}}{4}}[{\boldsymbol {\sigma }}_{x}{\boldsymbol {\sigma }}_{y}-{\boldsymbol {\sigma }}_{y}{\boldsymbol {\sigma }}_{x}]={\frac {i\hbar ^{2}}{2}}{\begin{pmatrix}1&0\\0&-1\\\end{pmatrix}}\leftrightarrow i\hbar s_{z}.$

It is shown in this manner that

$[s_{x},\,s_{y}]=i\hbar s_{z},\quad [s_{z},\,s_{x}]=i\hbar s_{y},\quad [s_{y},\,s_{z}]=i\hbar s_{x},$

which may be compared with the commutation relations of the orbital angular momenta given earlier.

Abstract angular momentum operators

Angular momentum operators are Hermitian operators j_x, j_y, and j_z,that satisfy the commutation relations

$[j_{k},j_{l}]=i\sum _{m=x,y,z}\varepsilon _{klm}j_{m},$

where $\varepsilon _{klm}$ is the Levi-Civita symbol. Together the three components define a vector operator $\mathbf {j}$. The square of the length of $\mathbf {j}$ is defined as

$\mathbf {j} ^{2}=j_{x}^{2}+j_{y}^{2}+j_{z}^{2}.$

We also define raising $(j_{+})$ and lowering $(j_{-})$ operators

$j_{\pm }=j_{x}\pm ij_{y}.\,$

Angular momentum states

It can be shown from the above definitions that j² commutes with j_x, j_y, and j_z

$[\mathbf {j} ^{2},j_{k}]=0\quad \mathrm {for} \;\;k=x,y,z.$

When two Hermitian operators commute a common set of eigenfunctions exists. Conventionally j² and j_z are chosen. From the commutation relations the possible eigenvalues can be found. The result is

$\mathbf {j} ^{2}|jm\rangle =j(j+1)|jm\rangle ,\qquad j=0,1/2,1,3/2,2,\ldots$

$j_{z}|jm\rangle =m|jm\rangle ,\qquad \quad m=-j,-j+1,\ldots ,j.$

The raising and lowering operators change the value of $m$

$j_{\pm }|jm\rangle =C_{\pm }(j,m)|jm\pm 1\rangle$

with

$C_{\pm }(j,m)={\sqrt {j(j+1)-m(m\pm 1)}}={\sqrt {(j\mp m)(j\pm m+1)}}.$

A (complex) phase factor could be included in the definition of $C_{\pm }(j,m)$ The choice made here is in agreement with the Condon and Shortley phase conventions. The angular momentum states must be orthogonal (because their eigenvalues with respect to a Hermitian operator are distinct) and they are assumed to be normalized

$\langle jm|j'm'\rangle =\delta _{j,j'}\delta _{m,m'}.$

References

(to be continued)