Commutation and anti-commutation relations

Anticommutation relations

They also satisfy the anticommutation relations:

${\displaystyle \{\sigma _{i},\sigma _{j}\}=2\delta _{ij}\,I,}$

where ${\displaystyle \{\sigma _{i},\sigma _{j}\}}$ is defined as ${\displaystyle \sigma _{i}\sigma _{j}+\sigma _{j}\sigma _{i},}$ and δ_ij is the Kronecker delta. I denotes the 2 × 2 identity matrix.

These anti-commutation relations make the Pauli matrices the generators of a representation of the Clifford algebra for ${\displaystyle \mathbb {R} ^{3},}$ denoted ${\displaystyle \mathrm {Cl} _{3}(\mathbb {R} ).}$

The usual construction of generators ${\textstyle \sigma _{ij}={\tfrac {1}{4}}\left[\sigma _{i},\sigma _{j}\right],}$ of ${\displaystyle {\mathfrak {so}}(3)}$ using the Clifford algebra recovers the commutation relations above, up to unimportant numerical factors.

A few explicit commutators and anti-commutators are given below as examples:

Commutators	Anticommutators
${\displaystyle {\begin{aligned}\left[\sigma _{1},\sigma _{1}\right]&=0\\\left[\sigma _{1},\sigma _{2}\right]&=2i\sigma _{3}\\\left[\sigma _{2},\sigma _{3}\right]&=2i\sigma _{1}\\\left[\sigma _{3},\sigma _{1}\right]&=2i\sigma _{2}\end{aligned}}}$	${\displaystyle {\begin{aligned}\left\{\sigma _{1},\sigma _{1}\right\}&=2I\\\left\{\sigma _{1},\sigma _{2}\right\}&=0\\\left\{\sigma _{1},\sigma _{3}\right\}&=0\\\left\{\sigma _{3},\sigma _{1}\right\}&=0\end{aligned}}}$

Eigenvectors and eigenvalues

Each of the (Hermitian) Pauli matrices has two eigenvalues, +1 and −1. The corresponding normalized eigenvectors are:

${\displaystyle {\begin{aligned}\psi _{x+}={\frac {1}{\sqrt {2\,}}}&{\begin{bmatrix}1\\1\end{bmatrix}}\;,&\psi _{x-}={\frac {1}{\sqrt {2\,}}}&{\begin{bmatrix}1\\-1\end{bmatrix}}\;,\\\psi _{y+}={\frac {1}{\sqrt {2\,}}}&{\begin{bmatrix}1\\i\end{bmatrix}}\;,&\psi _{y-}={\frac {1}{\sqrt {2\,}}}&{\begin{bmatrix}1\\-i\end{bmatrix}}\;,\\\psi _{z+}={}&{\begin{bmatrix}1\\0\end{bmatrix}}\;,&\psi _{z-}={}&{\begin{bmatrix}0\\1\end{bmatrix}}.\end{aligned}}}$

Completeness relation

Each component of ${\displaystyle \ {\vec {a}}\ }$ can be recovered from the matrix (see completeness relation below)

$${\displaystyle {\tfrac {1}{2}}\operatorname {tr} {\Bigl (}{\bigl (}{\vec {a}}\cdot {\vec {\sigma }}{\bigr )}{\vec {\sigma }}{\Bigr )}={\vec {a}}.}$$

This constitutes an inverse to the map ${\displaystyle {\vec {a}}\mapsto {\vec {a}}\cdot {\vec {\sigma }}}$, making it manifest that the map is a bijection.

Determinant

The norm is given by the determinant (up to a minus sign)

$${\displaystyle \det {\bigl (}{\vec {a}}\cdot {\vec {\sigma }}{\bigr )}=-{\vec {a}}\cdot {\vec {a}}=-\left|{\vec {a}}\right|^{2}.}$$

Then considering the conjugation action of an ${\displaystyle {\text{SU}}(2)}$ matrix ${\displaystyle U}$ on this space of matrices,

${\displaystyle U*{\vec {a}}\cdot {\vec {\sigma }}:=U\;{\vec {a}}\cdot {\vec {\sigma }}~U^{-1}\ ,}$

we find ${\displaystyle \ \det(U*{\vec {a}}\cdot {\vec {\sigma }})=\det({\vec {a}}\cdot {\vec {\sigma }})\ ,}$ and that ${\displaystyle \ U*{\vec {a}}\cdot {\vec {\sigma }}\ }$ is Hermitian and traceless. It then makes sense to define ${\displaystyle \ U*{\vec {a}}\cdot {\vec {\sigma }}={\vec {a}}'\cdot {\vec {\sigma }}\ }$ where ${\displaystyle \ {\vec {a}}'\ }$ has the same norm as ${\displaystyle \ {\vec {a}}\ ,}$ and therefore interpret ${\displaystyle \ U\ }$ as a rotation of three-dimensional space. In fact, it turns out that the special restriction on ${\displaystyle \ U\ }$ implies that the rotation is orientation preserving. This allows the definition of a map ${\displaystyle \ R:\mathrm {SU} (2)\rightarrow \mathrm {SO} (3)\ }$ given by

${\displaystyle U*{\vec {a}}\cdot {\vec {\sigma }}={\vec {a}}'\cdot {\vec {\sigma }}=:(R(U)\ {\vec {a}})\cdot {\vec {\sigma }}\ ,}$

where ${\displaystyle \ R(U)\in \mathrm {SO} (3).}$ This map is the concrete realization of the double cover of ${\displaystyle \ \mathrm {SO} (3)\ }$ by ${\displaystyle \ \mathrm {SU} (2)\ ,}$ and therefore shows that ${\displaystyle \ {\text{SU}}(2)\cong \mathrm {Spin} (3).}$ The components of ${\displaystyle R(U)}$ can be recovered using the tracing process above:

${\displaystyle R(U)_{ij}={\tfrac {1}{2}}\operatorname {tr} \left(\sigma _{i}U\sigma _{j}U^{-1}\right)}$

Cross-product

The cross-product is given by the matrix commutator (up to a factor of ${\displaystyle 2i}$)

$${\displaystyle \left[{\vec {a}}\cdot {\vec {\sigma }},{\vec {b}}\cdot {\vec {\sigma }}\right]=2i({\vec {a}}\times {\vec {b}})\cdot {\vec {\sigma }}.}$$

In fact, the existence of a norm follows from the fact that ${\displaystyle \mathbb {R} ^{3}}$ is a Lie algebra: see Killing form.

This cross-product can be used to prove the orientation-preserving property of the map above.

Eigenvalues and eigenvectors

The eigenvalues of ${\displaystyle \ {\vec {a}}\cdot {\vec {\sigma }}\ }$ are ${\displaystyle \ \pm |{\vec {a}}|.}$ This follows immediately from tracelessness and explicitly computing the determinant.

More abstractly, without computing the determinant, which requires explicit properties of the Pauli matrices, this follows from ${\displaystyle \ ({\vec {a}}\cdot {\vec {\sigma }})^{2}-|{\vec {a}}|^{2}=0\ ,}$ since this can be factorised into ${\displaystyle \ ({\vec {a}}\cdot {\vec {\sigma }}-|{\vec {a}}|)({\vec {a}}\cdot {\vec {\sigma }}+|{\vec {a}}|)=0.}$ A standard result in linear algebra (a linear map that satisfies a polynomial equation written in distinct linear factors is diagonal) means this implies ${\displaystyle \ {\vec {a}}\cdot {\vec {\sigma }}\ }$ is diagonal with possible eigenvalues ${\displaystyle \ \pm |{\vec {a}}|.}$ The tracelessness of ${\displaystyle \ {\vec {a}}\cdot {\vec {\sigma }}\ }$ means it has exactly one of each eigenvalue.

Its normalized eigenvectors are

$${\displaystyle \psi _{+}={\frac {1}{{\sqrt {2\left|{\vec {a}}\right|\ (a_{3}+\left|{\vec {a}}\right|)\ }}\ }}{\begin{bmatrix}a_{3}+\left|{\vec {a}}\right|\\a_{1}+ia_{2}\end{bmatrix}};\qquad \psi _{-}={\frac {1}{\sqrt {2|{\vec {a}}|(a_{3}+|{\vec {a}}|)}}}{\begin{bmatrix}ia_{2}-a_{1}\\a_{3}+|{\vec {a}}|\end{bmatrix}}~.}$$

These expressions become singular for ${\displaystyle a_{3}\to -1}$. They can be rescued by letting ${\displaystyle {\vec {a}}=(\epsilon ,0,-(1-\epsilon ^{2}/2))}$ and taking the limit ${\displaystyle \epsilon \to 0}$, which yields the correct eigenvectors (0,1) and (1,0) of ${\displaystyle \sigma _{z}}$.

Alternatively, one may use spherical coordinates ${\displaystyle {\vec {a}}=a(\sin \vartheta \cos \varphi ,\sin \vartheta \sin \varphi ,\cos \vartheta )}$ to obtain the eigenvectors ${\displaystyle \psi _{+}=(\cos(\vartheta /2),\sin(\vartheta /2)\exp(i\varphi ))}$ and ${\displaystyle \psi _{-}=(-\sin(\vartheta /2)\exp(-i\varphi ),\cos(\vartheta /2))}$.

Pauli 4-vector

The Pauli 4-vector, used in spinor theory, is written ${\displaystyle \ \sigma ^{\mu }\ }$ with components

${\displaystyle \sigma ^{\mu }=(I,{\vec {\sigma }}).}$

This defines a map from ${\displaystyle \mathbb {R} ^{1,3}}$ to the vector space of Hermitian matrices,

${\displaystyle x_{\mu }\mapsto x_{\mu }\sigma ^{\mu }\ ,}$

which also encodes the Minkowski metric (with mostly minus convention) in its determinant:

${\displaystyle \det(x_{\mu }\sigma ^{\mu })=\eta (x,x).}$

This 4-vector also has a completeness relation. It is convenient to define a second Pauli 4-vector

${\displaystyle {\bar {\sigma }}^{\mu }=(I,-{\vec {\sigma }}).}$

and allow raising and lowering using the Minkowski metric tensor. The relation can then be written

$${\displaystyle x_{\nu }={\tfrac {1}{2}}\operatorname {tr} {\Bigl (}{\bar {\sigma }}_{\nu }{\bigl (}x_{\mu }\sigma ^{\mu }{\bigr )}{\Bigr )}.}$$

Similarly to the Pauli 3-vector case, we can find a matrix group that acts as isometries on ${\displaystyle \ \mathbb {R} ^{1,3}\$ ;} in this case the matrix group is ${\displaystyle \ \mathrm {SL} (2,\mathbb {C} )\ ,}$ and this shows ${\displaystyle \ \mathrm {SL} (2,\mathbb {C} )\cong \mathrm {Spin} (1,3).}$ Similarly to above, this can be explicitly realized for ${\displaystyle \ S\in \mathrm {SL} (2,\mathbb {C} )\ }$ with components

${\displaystyle \Lambda (S)^{\mu }{}_{\nu }={\tfrac {1}{2}}\operatorname {tr} \left({\bar {\sigma }}_{\nu }S\sigma ^{\mu }S^{\dagger }\right).}$

In fact, the determinant property follows abstractly from trace properties of the ${\displaystyle \ \sigma ^{\mu }.}$ For ${\displaystyle \ 2\times 2\ }$ matrices, the following identity holds:

${\displaystyle \det(A+B)=\det(A)+\det(B)+\operatorname {tr} (A)\operatorname {tr} (B)-\operatorname {tr} (AB).}$

That is, the 'cross-terms' can be written as traces. When ${\displaystyle \ A,B\ }$ are chosen to be different ${\displaystyle \ \sigma ^{\mu }\ ,}$ the cross-terms vanish. It then follows, now showing summation explicitly, ${\textstyle \det \left(\sum _{\mu }x_{\mu }\sigma ^{\mu }\right)=\sum _{\mu }\det \left(x_{\mu }\sigma ^{\mu }\right).}$ Since the matrices are ${\displaystyle \ 2\times 2\ ,}$ this is equal to ${\textstyle \sum _{\mu }x_{\mu }^{2}\det(\sigma ^{\mu })=\eta (x,x).}$

Relation to dot and cross product

Pauli vectors elegantly map these commutation and anticommutation relations to corresponding vector products. Adding the commutator to the anticommutator gives

${\displaystyle {\begin{aligned}\left[\sigma _{j},\sigma _{k}\right]+\{\sigma _{j},\sigma _{k}\}&=(\sigma _{j}\sigma _{k}-\sigma _{k}\sigma _{j})+(\sigma _{j}\sigma _{k}+\sigma _{k}\sigma _{j})\\2i\varepsilon _{jk\ell }\,\sigma _{\ell }+2\delta _{jk}I&=2\sigma _{j}\sigma _{k}\end{aligned}}}$

so that,

Contracting each side of the equation with components of two 3-vectors a_p and b_q (which commute with the Pauli matrices, i.e., a_pσ_q = σ_qa_p) for each matrix σ_q and vector component a_p (and likewise with b_q) yields

${\displaystyle ~~{\begin{aligned}a_{j}b_{k}\sigma _{j}\sigma _{k}&=a_{j}b_{k}\left(i\varepsilon _{jk\ell }\,\sigma _{\ell }+\delta _{jk}I\right)\\a_{j}\sigma _{j}b_{k}\sigma _{k}&=i\varepsilon _{jk\ell }\,a_{j}b_{k}\sigma _{\ell }+a_{j}b_{k}\delta _{jk}I\end{aligned}}.~}$

Finally, translating the index notation for the dot product and cross product results in

If i is identified with the pseudoscalar σ_xσ_yσ_z then the right hand side becomes ${\displaystyle a\cdot b+a\wedge b}$, which is also the definition for the product of two vectors in geometric algebra.

If we define the spin operator as J = ħ/2σ, then J satisfies the commutation relation:

$${\displaystyle \mathbf {J} \times \mathbf {J} =i\hbar \mathbf {J} }$$

Or equivalently, the Pauli vector satisfies:

$${\displaystyle {\frac {\vec {\sigma }}{2}}\times {\frac {\vec {\sigma }}{2}}=i{\frac {\vec {\sigma }}{2}}}$$

Some trace relations

The following traces can be derived using the commutation and anticommutation relations.

${\displaystyle {\begin{aligned}\operatorname {tr} \left(\sigma _{j}\right)&=0\\\operatorname {tr} \left(\sigma _{j}\sigma _{k}\right)&=2\delta _{jk}\\\operatorname {tr} \left(\sigma _{j}\sigma _{k}\sigma _{\ell }\right)&=2i\varepsilon _{jk\ell }\\\operatorname {tr} \left(\sigma _{j}\sigma _{k}\sigma _{\ell }\sigma _{m}\right)&=2\left(\delta _{jk}\delta _{\ell m}-\delta _{j\ell }\delta _{km}+\delta _{jm}\delta _{k\ell }\right)\end{aligned}}}$

If the matrix σ₀ = I is also considered, these relationships become

$${\displaystyle {\begin{aligned}\operatorname {tr} \left(\sigma _{\alpha }\right)&=2\delta _{0\alpha }\\\operatorname {tr} \left(\sigma _{\alpha }\sigma _{\beta }\right)&=2\delta _{\alpha \beta }\\\operatorname {tr} \left(\sigma _{\alpha }\sigma _{\beta }\sigma _{\gamma }\right)&=2\sum _{(\alpha \beta \gamma )}\delta _{\alpha \beta }\delta _{0\gamma }-4\delta _{0\alpha }\delta _{0\beta }\delta _{0\gamma }+2i\varepsilon _{0\alpha \beta \gamma }\\\operatorname {tr} \left(\sigma _{\alpha }\sigma _{\beta }\sigma _{\gamma }\sigma _{\mu }\right)&=2\left(\delta _{\alpha \beta }\delta _{\gamma \mu }-\delta _{\alpha \gamma }\delta _{\beta \mu }+\delta _{\alpha \mu }\delta _{\beta \gamma }\right)+4\left(\delta _{\alpha \gamma }\delta _{0\beta }\delta _{0\mu }+\delta _{\beta \mu }\delta _{0\alpha }\delta _{0\gamma }\right)-8\delta _{0\alpha }\delta _{0\beta }\delta _{0\gamma }\delta _{0\mu }+2i\sum _{(\alpha \beta \gamma \mu )}\varepsilon _{0\alpha \beta \gamma }\delta _{0\mu }\end{aligned}}}$$

where Greek indices α, β, γ and μ assume values from {0, x, y, z} and the notation ${\textstyle \sum _{(\alpha \ldots )}}$ is used to denote the sum over the cyclic permutation of the included indices.

Exponential of a Pauli vector

For

${\displaystyle {\vec {a}}=a{\hat {n}},\quad |{\hat {n}}|=1,}$

one has, for even powers, 2p, p = 0, 1, 2, 3, ...

${\displaystyle ({\hat {n}}\cdot {\vec {\sigma }})^{2p}=I,}$

which can be shown first for the p = 1 case using the anticommutation relations. For convenience, the case p = 0 is taken to be I by convention.

For odd powers, 2q + 1, q = 0, 1, 2, 3, ...

${\displaystyle \left({\hat {n}}\cdot {\vec {\sigma }}\right)^{2q+1}={\hat {n}}\cdot {\vec {\sigma }}\,.}$

Matrix exponentiating, and using the Taylor series for sine and cosine,

${\displaystyle {\begin{aligned}e^{ia\left({\hat {n}}\cdot {\vec {\sigma }}\right)}&=\sum _{k=0}^{\infty }{\frac {i^{k}\left[a\left({\hat {n}}\cdot {\vec {\sigma }}\right)\right]^{k}}{k!}}\\&=\sum _{p=0}^{\infty }{\frac {(-1)^{p}(a{\hat {n}}\cdot {\vec {\sigma }})^{2p}}{(2p)!}}+i\sum _{q=0}^{\infty }{\frac {(-1)^{q}(a{\hat {n}}\cdot {\vec {\sigma }})^{2q+1}}{(2q+1)!}}\\&=I\sum _{p=0}^{\infty }{\frac {(-1)^{p}a^{2p}}{(2p)!}}+i({\hat {n}}\cdot {\vec {\sigma }})\sum _{q=0}^{\infty }{\frac {(-1)^{q}a^{2q+1}}{(2q+1)!}}\\\end{aligned}}}$.

In the last line, the first sum is the cosine, while the second sum is the sine; so, finally,

which is analogous to Euler's formula, extended to quaternions.

Note that

${\displaystyle \det[ia({\hat {n}}\cdot {\vec {\sigma }})]=a^{2}}$,

while the determinant of the exponential itself is just 1, which makes it the generic group element of SU(2).

A more abstract version of formula (2) for a general 2 × 2 matrix can be found in the article on matrix exponentials. A general version of (2) for an analytic (at a and −a) function is provided by application of Sylvester's formula,^[3]

${\displaystyle f(a({\hat {n}}\cdot {\vec {\sigma }}))=I{\frac {f(a)+f(-a)}{2}}+{\hat {n}}\cdot {\vec {\sigma }}{\frac {f(a)-f(-a)}{2}}.}$

The group composition law of SU(2)

A straightforward application of formula (2) provides a parameterization of the composition law of the group SU(2).^{[lower-alpha 3]} One may directly solve for c in

$${\displaystyle {\begin{aligned}e^{ia\left({\hat {n}}\cdot {\vec {\sigma }}\right)}e^{ib\left({\hat {m}}\cdot {\vec {\sigma }}\right)}&=I\left(\cos a\cos b-{\hat {n}}\cdot {\hat {m}}\sin a\sin b\right)+i\left({\hat {n}}\sin a\cos b+{\hat {m}}\sin b\cos a-{\hat {n}}\times {\hat {m}}~\sin a\sin b\right)\cdot {\vec {\sigma }}\\&=I\cos {c}+i\left({\hat {k}}\cdot {\vec {\sigma }}\right)\sin c\\&=e^{ic\left({\hat {k}}\cdot {\vec {\sigma }}\right)},\end{aligned}}}$$

which specifies the generic group multiplication, where, manifestly,

$${\displaystyle \cos c=\cos a\cos b-{\hat {n}}\cdot {\hat {m}}\sin a\sin b~,}$$

the spherical law of cosines. Given c, then,

$${\displaystyle {\hat {k}}={\frac {1}{\sin c}}\left({\hat {n}}\sin a\cos b+{\hat {m}}\sin b\cos a-{\hat {n}}\times {\hat {m}}\sin a\sin b\right).}$$

Consequently, the composite rotation parameters in this group element (a closed form of the respective BCH expansion in this case) simply amount to^[4]

$${\displaystyle e^{ic{\hat {k}}\cdot {\vec {\sigma }}}=\exp \left(i{\frac {c}{\sin c}}\left({\hat {n}}\sin a\cos b+{\hat {m}}\sin b\cos a-{\hat {n}}\times {\hat {m}}~\sin a\sin b\right)\cdot {\vec {\sigma }}\right).}$$

(Of course, when ${\displaystyle {\hat {n}}}$ is parallel to ${\displaystyle {\hat {m}}}$, so is ${\displaystyle {\hat {k}}}$, and c = a + b.)

See also: Rotation formalisms in three dimensions § Rodrigues vector, and Spinor § Three dimensions

Adjoint action

It is also straightforward to likewise work out the adjoint action on the Pauli vector, namely rotation of any angle ${\displaystyle a}$ along any axis ${\displaystyle {\hat {n}}}$:

$${\displaystyle R_{n}(-a)~{\vec {\sigma }}~R_{n}(a)=e^{i{\frac {a}{2}}\left({\hat {n}}\cdot {\vec {\sigma }}\right)}~{\vec {\sigma }}~e^{-i{\frac {a}{2}}\left({\hat {n}}\cdot {\vec {\sigma }}\right)}={\vec {\sigma }}\cos(a)+{\hat {n}}\times {\vec {\sigma }}~\sin(a)+{\hat {n}}~{\hat {n}}\cdot {\vec {\sigma }}~(1-\cos(a))~.}$$

Taking the dot product of any unit vector with the above formula generates the expression of any single qubit operator under any rotation. For example, it can be shown that ${\textstyle R_{y}{\mathord {\left(-{\frac {\pi }{2}}\right)}}\,\sigma _{x}\,R_{y}{\mathord {\left({\frac {\pi }{2}}\right)}}={\hat {x}}\cdot \left({\hat {y}}\times {\vec {\sigma }}\right)=\sigma _{z}}$.

See also: Rodrigues' rotation formula

Completeness relation

An alternative notation that is commonly used for the Pauli matrices is to write the vector index k in the superscript, and the matrix indices as subscripts, so that the element in row α and column β of the k-th Pauli matrix is σ ^k_αβ.

In this notation, the completeness relation for the Pauli matrices can be written

${\displaystyle {\vec {\sigma }}_{\alpha \beta }\cdot {\vec {\sigma }}_{\gamma \delta }\equiv \sum _{k=1}^{3}\sigma _{\alpha \beta }^{k}\,\sigma _{\gamma \delta }^{k}=2\,\delta _{\alpha \delta }\,\delta _{\beta \gamma }-\delta _{\alpha \beta }\,\delta _{\gamma \delta }.}$

Proof

The fact that the Pauli matrices, along with the identity matrix I, form an orthogonal basis for the Hilbert space of all 2 × 2 complex matrices means that we can express any matrix M as

$${\displaystyle M=c\,I+\sum _{k}a_{k}\,\sigma ^{k}}$$

where c is a complex number, and a is a 3-component, complex vector. It is straightforward to show, using the properties listed above, that

$${\displaystyle \operatorname {tr} \left(\sigma ^{j}\,\sigma ^{k}\right)=2\,\delta _{jk}}$$

where "tr" denotes the trace, and hence that

$${\displaystyle {\begin{aligned}c&={}{\tfrac {1}{2}}\,\operatorname {tr} \,M\,,{\begin{aligned}&&a_{k}&={\tfrac {1}{2}}\,\operatorname {tr} \,\sigma ^{k}\,M.\end{aligned}}\\[3pt]\therefore ~~2\,M&=I\,\operatorname {tr} \,M+\sum _{k}\sigma ^{k}\,\operatorname {tr} \,\sigma ^{k}M~,\end{aligned}}}$$

which can be rewritten in terms of matrix indices as

$${\displaystyle 2\,M_{\alpha \beta }=\delta _{\alpha \beta }\,M_{\gamma \gamma }+\sum _{k}\sigma _{\alpha \beta }^{k}\,\sigma _{\gamma \delta }^{k}\,M_{\delta \gamma }~,}$$

where summation over the repeated indices is implied γ and δ. Since this is true for any choice of the matrix M, the completeness relation follows as stated above. Q.E.D.

As noted above, it is common to denote the 2 × 2 unit matrix by σ₀, so σ⁰_αβ = δ_αβ. The completeness relation can alternatively be expressed as

$${\displaystyle \sum _{k=0}^{3}\sigma _{\alpha \beta }^{k}\,\sigma _{\gamma \delta }^{k}=2\,\delta _{\alpha \delta }\,\delta _{\beta \gamma }~.}$$

The fact that any Hermitian complex 2 × 2 matrices can be expressed in terms of the identity matrix and the Pauli matrices also leads to the Bloch sphere representation of 2 × 2 mixed states’ density matrix, (positive semidefinite 2 × 2 matrices with unit trace. This can be seen by first expressing an arbitrary Hermitian matrix as a real linear combination of {σ₀, σ₁, σ₂, σ₃} as above, and then imposing the positive-semidefinite and trace 1 conditions.

For a pure state, in polar coordinates,

$${\displaystyle {\vec {a}}={\begin{pmatrix}\sin \theta \cos \phi &\sin \theta \sin \phi &\cos \theta \end{pmatrix}},}$$

the idempotent density matrix

$${\displaystyle {\tfrac {1}{2}}\left(\mathbf {1} +{\vec {a}}\cdot {\vec {\sigma }}\right)={\begin{pmatrix}\cos ^{2}\left({\frac {\,\theta \,}{2}}\right)&e^{-i\,\phi }\sin \left({\frac {\,\theta \,}{2}}\right)\cos \left({\frac {\,\theta \,}{2}}\right)\\e^{+i\,\phi }\sin \left({\frac {\,\theta \,}{2}}\right)\cos \left({\frac {\,\theta \,}{2}}\right)&\sin ^{2}\left({\frac {\,\theta \,}{2}}\right)\end{pmatrix}}}$$

acts on the state eigenvector ${\displaystyle {\begin{pmatrix}\cos \left({\frac {\,\theta \,}{2}}\right)&e^{+i\phi }\,\sin \left({\frac {\,\theta \,}{2}}\right)\end{pmatrix}}}$ with eigenvalue +1, hence it acts like a projection operator.

Relation with the permutation operator

Let P_jk be the transposition (also known as a permutation) between two spins σ_j and σ_k living in the tensor product space ${\displaystyle \mathbb {C} ^{2}\otimes \mathbb {C} ^{2}}$,

${\displaystyle P_{jk}\left|\sigma _{j}\sigma _{k}\right\rangle =\left|\sigma _{k}\sigma _{j}\right\rangle .}$

This operator can also be written more explicitly as Dirac's spin exchange operator,

${\displaystyle P_{jk}={\frac {1}{2}}\,\left({\vec {\sigma }}_{j}\cdot {\vec {\sigma }}_{k}+1\right)~.}$

Its eigenvalues are therefore^{[lower-alpha 4]} 1 or −1. It may thus be utilized as an interaction term in a Hamiltonian, splitting the energy eigenvalues of its symmetric versus antisymmetric eigenstates.

SO(3)

The Lie algebra ${\displaystyle {\mathfrak {su}}(2)}$ is isomorphic to the Lie algebra ${\displaystyle {\mathfrak {so}}(3)}$, which corresponds to the Lie group SO(3), the group of rotations in three-dimensional space. In other words, one can say that the iσ_j are a realization (and, in fact, the lowest-dimensional realization) of infinitesimal rotations in three-dimensional space. However, even though ${\displaystyle {\mathfrak {su}}(2)}$ and ${\displaystyle {\mathfrak {so}}(3)}$ are isomorphic as Lie algebras, SU(2) and SO(3) are not isomorphic as Lie groups. SU(2) is actually a double cover of SO(3), meaning that there is a two-to-one group homomorphism from SU(2) to SO(3), see relationship between SO(3) and SU(2).

Quaternions

The real linear span of {I, iσ₁, iσ₂, iσ₃} is isomorphic to the real algebra of quaternions, ${\displaystyle \mathbb {H} }$, represented by the span of the basis vectors ${\displaystyle \left\{\;\mathbf {1} ,\,\mathbf {i} ,\,\mathbf {j} ,\,\mathbf {k} \;\right\}.}$ The isomorphism from ${\displaystyle \mathbb {H} }$ to this set is given by the following map (notice the reversed signs for the Pauli matrices):

$${\displaystyle \mathbf {1} \mapsto I,\quad \mathbf {i} \mapsto -\sigma _{2}\sigma _{3}=-i\,\sigma _{1},\quad \mathbf {j} \mapsto -\sigma _{3}\sigma _{1}=-i\,\sigma _{2},\quad \mathbf {k} \mapsto -\sigma _{1}\sigma _{2}=-i\,\sigma _{3}.}$$

Alternatively, the isomorphism can be achieved by a map using the Pauli matrices in reversed order,^[5]

${\displaystyle \mathbf {1} \mapsto I,\quad \mathbf {i} \mapsto i\,\sigma _{3}\,,\quad \mathbf {j} \mapsto i\,\sigma _{2}\,,\quad \mathbf {k} \mapsto i\,\sigma _{1}~.}$

As the set of versors U ⊂ ${\displaystyle \mathbb {H} }$ forms a group isomorphic to SU(2), U gives yet another way of describing SU(2). The two-to-one homomorphism from SU(2) to SO(3) may be given in terms of the Pauli matrices in this formulation.

Classical mechanics

In classical mechanics, Pauli matrices are useful in the context of the Cayley-Klein parameters.^[6] The matrix P corresponding to the position ${\displaystyle {\vec {x}}}$ of a point in space is defined in terms of the above Pauli vector matrix,

${\displaystyle P={\vec {x}}\cdot {\vec {\sigma }}=x\,\sigma _{x}+y\,\sigma _{y}+z\,\sigma _{z}.}$

Consequently, the transformation matrix Q_θ for rotations about the x-axis through an angle θ may be written in terms of Pauli matrices and the unit matrix as^[6]

${\displaystyle Q_{\theta }={\boldsymbol {1}}\,\cos {\frac {\theta }{2}}+i\,\sigma _{x}\sin {\frac {\theta }{2}}.}$

Similar expressions follow for general Pauli vector rotations as detailed above.

Quantum mechanics

In quantum mechanics, each Pauli matrix is related to an angular momentum operator that corresponds to an observable describing the spin of a spin 1⁄2 particle, in each of the three spatial directions. As an immediate consequence of the Cartan decomposition mentioned above, iσ_j are the generators of a projective representation (spin representation) of the rotation group SO(3) acting on non-relativistic particles with spin 1⁄2. The states of the particles are represented as two-component spinors. In the same way, the Pauli matrices are related to the isospin operator.

An interesting property of spin 1⁄2 particles is that they must be rotated by an angle of 4π in order to return to their original configuration. This is due to the two-to-one correspondence between SU(2) and SO(3) mentioned above, and the fact that, although one visualizes spin up/down as the north–south pole on the 2-sphere S², they are actually represented by orthogonal vectors in the two-dimensional complex Hilbert space.

For a spin 1⁄2 particle, the spin operator is given by J = ħ/2σ, the fundamental representation of SU(2). By taking Kronecker products of this representation with itself repeatedly, one may construct all higher irreducible representations. That is, the resulting spin operators for higher spin systems in three spatial dimensions, for arbitrarily large j, can be calculated using this spin operator and ladder operators. They can be found in Rotation group SO(3) § A note on Lie algebras. The analog formula to the above generalization of Euler's formula for Pauli matrices, the group element in terms of spin matrices, is tractable, but less simple.^[7]

Also useful in the quantum mechanics of multiparticle systems, the general Pauli group G_n is defined to consist of all n-fold tensor products of Pauli matrices.

Relativistic quantum mechanics

In relativistic quantum mechanics, the spinors in four dimensions are 4 × 1 (or 1 × 4) matrices. Hence the Pauli matrices or the Sigma matrices operating on these spinors have to be 4 × 4 matrices. They are defined in terms of 2 × 2 Pauli matrices as

${\displaystyle {\mathsf {\Sigma }}_{k}={\begin{pmatrix}{\mathsf {\sigma }}_{k}&0\\0&{\mathsf {\sigma }}_{k}\end{pmatrix}}.}$

It follows from this definition that the ${\displaystyle \ {\mathsf {\Sigma }}_{k}\ }$ matrices have the same algebraic properties as the σ_k matrices.

However, relativistic angular momentum is not a three-vector, but a second order four-tensor. Hence ${\displaystyle \ {\mathsf {\Sigma }}_{k}\ }$ needs to be replaced by Σ_μν , the generator of Lorentz transformations on spinors. By the antisymmetry of angular momentum, the Σ_μν are also antisymmetric. Hence there are only six independent matrices.

The first three are the ${\displaystyle \ \Sigma _{k\ell }\equiv \epsilon _{jk\ell }{\mathsf {\Sigma }}_{j}.}$ The remaining three, ${\displaystyle \ -i\ \Sigma _{0k}\equiv {\mathsf {\alpha }}_{k}\ ,}$ where the Dirac α_k matrices are defined as

${\displaystyle {\mathsf {\alpha }}_{k}={\begin{pmatrix}0&{\mathsf {\sigma }}_{k}\\{\mathsf {\sigma }}_{k}&0\end{pmatrix}}.}$

The relativistic spin matrices Σ_μν are written in compact form in terms of commutator of gamma matrices as

${\displaystyle \Sigma _{\mu \nu }={\frac {i}{2}}{\bigl [}\gamma _{\mu },\gamma _{\nu }{\bigr ]}.}$

Quantum information

In quantum information, single-qubit quantum gates are 2 × 2 unitary matrices. The Pauli matrices are some of the most important single-qubit operations. In that context, the Cartan decomposition given above is called the "Z–Y decomposition of a single-qubit gate". Choosing a different Cartan pair gives a similar "X–Y decomposition of a single-qubit gate.