Pauli matrices

In mathematical physics and mathematics, the Pauli matrices are a set of three $2 \times 2$ complex matrices which are Hermitian and unitary.^[1] Usually indicated by the Greek letter sigma ( $σ$ ), they are occasionally denoted by tau ( $τ$ ) when used in connection with isospin symmetries. They are

{\begin{aligned}\sigma _{1}=\sigma _{x}&={\begin{pmatrix}0&1\\1&0\end{pmatrix}}\\\sigma _{2}=\sigma _{y}&={\begin{pmatrix}0&-i\\i&0\end{pmatrix}}\\\sigma _{3}=\sigma _{z}&={\begin{pmatrix}1&0\\0&-1\end{pmatrix}}\,.\end{aligned}}

These matrices are named after the physicist Wolfgang Pauli. In quantum mechanics, they occur in the Pauli equation which takes into account the interaction of the spin of a particle with an external electromagnetic field.

Each Pauli matrix is Hermitian, and together with the identity matrix $I$ (sometimes considered as the zeroth Pauli matrix $σ 0$ ), the Pauli matrices (multiplied by real coefficients) form a basis for the vector space of $2 \times 2$ Hermitian matrices.

Hermitian operators represent observables, so the Pauli matrices span the space of observables of the $2$ -dimensional complex Hilbert space. In the context of Pauli's work, $σ k$ represents the observable corresponding to spin along the $k$ th coordinate axis in three-dimensional Euclidean space $ℝ 3$ .

The Pauli matrices (after multiplication by $i$ to make them anti-Hermitian), also generate transformations in the sense of Lie algebras: the matrices $iσ 1, iσ 2, iσ 3$ form a basis for $su (2)$ , which exponentiates to the special unitary group SU(2). The algebra generated by the three matrices $σ 1, σ 2, σ 3$ is isomorphic to the Clifford algebra of $ℝ 3$ , called the algebra of physical space.

Algebraic properties

All three of the Pauli matrices can be compacted into a single expression:

\sigma _{a}={\begin{pmatrix}\delta _{{a3}}&\delta _{{a1}}-i\delta _{{a2}}\\\delta _{{a1}}+i\delta _{{a2}}&-\delta _{{a3}}\end{pmatrix}}

where $i = \sqrt -1$ is the imaginary unit, and $δ ab$ is the Kronecker delta, which equals +1 if $a = b$ and 0 otherwise. This expression is useful for "selecting" any one of the matrices numerically by substituting values of $a = 1, 2, 3$ , in turn useful when any of the matrices (but no particular one) is to be used in algebraic manipulations.

The matrices are involutory:

\sigma_1^2 = \sigma_2^2 = \sigma_3^2 = -i\sigma_1 \sigma_2 \sigma_3 = \begin{pmatrix} 1&0\\0&1\end{pmatrix} = I

where $I$ is the identity matrix.

The determinants and traces of the Pauli matrices are:

{\begin{aligned}\det \sigma _{i}&=-1,\\\operatorname {Tr}\sigma _{i}&=0.\end{aligned}}

From above we can deduce that the eigenvalues of each $σ i$ are $\pm1$ .

Together with the $2 \times 2$ identity matrix $I$ (sometimes written as $σ 0$ ), the Pauli matrices form an orthogonal basis, in the sense of Hilbert–Schmidt, for the real Hilbert space of $2 \times 2$ complex Hermitian matrices, or the complex Hilbert space of all $2 \times 2$ matrices.

Eigenvectors and eigenvalues

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

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

Pauli vector

The Pauli vector is defined by^{[nb 1]}

\vec{\sigma} = \sigma_1 \hat{x} + \sigma_2 \hat{y} + \sigma_3 \hat{z} \,

and provides a mapping mechanism from a vector basis to a Pauli matrix basis^[2] as follows,

\begin{align} \vec{a} \cdot \vec{\sigma} &= (a_i \hat{x}_i) \cdot (\sigma_j \hat{x}_j ) \\ &= a_i \sigma_j \hat{x}_i \cdot \hat{x}_j \\ &= a_i \sigma_j \delta_{ij} \\ &= a_i \sigma_i =\begin{pmatrix} a_3&a_1-ia_2\\a_1+ia_2&-a_3\end{pmatrix} \end{align}

using the summation convention. Further,

\det {\vec {a}}\cdot {\vec {\sigma }}=-{\vec {a}}\cdot {\vec {a}}=-|{\vec {a}}|^{2},

and also (see completeness, below)

{\frac {1}{2}}{\mathrm {tr}}[({\vec {a}}\cdot {\vec {\sigma }}){\vec {\sigma }}]={\vec {a}}.

Its (unnormalized) eigenvectors are $\psi _{+}={\begin{pmatrix}a_{3}+|{\vec {a}}|\\a_{1}+ia_{2}\end{pmatrix}};\qquad \psi _{-}={\begin{pmatrix}ia_{2}-a_{1}\\a_{3}+|{\vec {a}}|\end{pmatrix}}.$

Commutation relations

The Pauli matrices obey the following commutation relations:

[\sigma_a, \sigma_b] = 2 i \varepsilon_{a b c}\,\sigma_c \, ,

and anticommutation relations:

\{\sigma_a, \sigma_b\} = 2 \delta_{a b}\,I.

where the structure constant $ε abc$ is the Levi-Civita symbol, Einstein summation notation is used, $δ ab$ is the Kronecker delta, and $I$ is the $2 \times 2$ identity matrix.

For example,

{\begin{aligned}\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}\,\\\left[\sigma _{1},\sigma _{1}\right]&=0\,\\\left\{\sigma _{1},\sigma _{1}\right\}&=2I\,\\\left\{\sigma _{1},\sigma _{2}\right\}&=0\,.\\\end{aligned}}

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

{\begin{aligned}\left[\sigma _{a},\sigma _{b}\right]+\{\sigma _{a},\sigma _{b}\}&=(\sigma _{a}\sigma _{b}-\sigma _{b}\sigma _{a})+(\sigma _{a}\sigma _{b}+\sigma _{b}\sigma _{a})\\2i\varepsilon _{abc}\,\sigma _{c}+2\delta _{ab}I&=2\sigma _{a}\sigma _{b}\end{aligned}}

so that,

$\sigma _{a}\sigma _{b}=\delta _{ab}I+i\varepsilon _{abc}\,\sigma _{c}~.$

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., $a p σ q = σ q a p)$ for each matrix $σ q$ and vector component $a p$ (and likewise with $b q$ ), and relabeling indices $a, b, c \to p, q, r$ , to prevent notational conflicts, yields

{\begin{aligned}a_{p}b_{q}\sigma _{p}\sigma _{q}&=a_{p}b_{q}\left(i\varepsilon _{pqr}\,\sigma _{r}+\delta _{pq}I\right)\\a_{p}\sigma _{p}b_{q}\sigma _{q}&=i\varepsilon _{pqr}\,a_{p}b_{q}\sigma _{r}+a_{p}b_{q}\delta _{pq}I~.\end{aligned}}

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

$(\vec{a} \cdot \vec{\sigma})(\vec{b} \cdot \vec{\sigma}) = (\vec{a} \cdot \vec{b}) \, I + i ( \vec{a} \times \vec{b} )\cdot \vec{\sigma}$

(1 )

Some trace relations

Following traces can be derived using the commutation and anticommutation relations.

tr(\sigma _{a})=0

tr(\sigma _{a}\sigma _{b})=2\delta _{ab}

tr(\sigma _{a}\sigma _{b}\sigma _{c})=2i\epsilon _{abc}

tr(\sigma _{a}\sigma _{b}\sigma _{c}\sigma _{d})=2(\delta _{ab}\delta _{cd}-\delta _{ac}\delta _{bd}+\delta _{ad}\delta _{bc})

Exponential of a Pauli vector

For

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

one has, for even powers,

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

which can be shown first for the $n = 1$ case using the anticommutation relations.

Thus, for odd powers,

(\hat{n} \cdot \vec{\sigma})^{2n+1} = \hat{n} \cdot \vec{\sigma} \, .

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

\begin{align} e^{i a(\hat{n} \cdot \vec{\sigma})} &= \sum_{n=0}^\infty{\frac{i^n \left[a (\hat{n} \cdot \vec{\sigma})\right]^n}{n!}} \\ &= \sum_{n=0}^\infty{\frac{(-1)^n (a\hat{n}\cdot \vec{\sigma})^{2n}}{(2n)!}} + i\sum_{n=0}^\infty{\frac{(-1)^n (a\hat{n}\cdot \vec{\sigma})^{2n + 1}}{(2n + 1)!}} \\ &= I\sum_{n=0}^\infty{\frac{(-1)^n a^{2n}}{(2n)!}} + i (\hat{n}\cdot \vec{\sigma}) \sum_{n=0}^\infty{\frac{(-1)^n a^{2n+1}}{(2n + 1)!}}\\ \end{align}

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

$e^{i a(\hat{n} \cdot \vec{\sigma})} = I\cos{a} + i (\hat{n} \cdot \vec{\sigma}) \sin{a} \,$

(2 )

which is analogous to Euler's formula. Note

\det[i a(\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 $2 \times 2$ 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]

f(a(\hat{n} \cdot \vec{\sigma})) = I\frac{f(a)+f(-a)}{2} + i (\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 $SU(2)$ .^{[nb 2]} One may directly solve for $c$ in

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

which specifies the generic group multiplication, where, manifestly,

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

the spherical law of cosines. Given $c$ , then,

{\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]

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

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

The fact that any $2 \times 2$ complex Hermitian matrices can be expressed in terms of the identity matrix and the Pauli matrices also leads to the Bloch sphere representation of $2 \times 2$ mixed states' density matrix, ( $2 \times 2$ positive semidefinite matrices with trace $1$ ). This can be seen by simply first writing an arbitrary Hermitian matrix as a real linear combination of ${σ 0, σ 1, σ 2, σ 3}$ as above, and then imposing the positive-semidefinite and trace $1$ conditions.

Completeness relation

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

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

{\vec {\sigma }}_{\alpha \beta }\cdot {\vec {\sigma }}_{\gamma \delta }\equiv \sum _{i=1}^{3}\sigma _{\alpha \beta }^{i}\sigma _{\gamma \delta }^{i}=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 complex Hilbert space of all 2 × 2 matrices means that we can express any matrix M as

M = c I + \sum_i a_i \sigma^i

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

\mathrm{tr}\, \sigma^i\sigma^j = 2\delta_{ij}

where "tr" denotes the trace, and hence that

c=\frac{1}{2}\mathrm{tr}\,M

and

a_{i}={\frac {1}{2}}\mathrm {tr} \,\sigma ^{i}M~.

\therefore ~~2M=I\mathrm {tr} \,M+\sum _{i}\sigma ^{i}\mathrm {tr} \,\sigma ^{i}M~,

which can be rewritten in terms of matrix indices as

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

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

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

\sum _{i=0}^{3}\sigma _{\alpha \beta }^{i}\sigma _{\gamma \delta }^{i}=2\delta _{\alpha \delta }\delta _{\beta \gamma }~.

Relation with the permutation operator

Let $P ij$ be the transposition (also known as a permutation) between two spins $σ i$ and $σ j$ living in the tensor product space $ℂ 2 \otimes ℂ 2$ ,

P_{ij}|\sigma_i \sigma_j\rangle = |\sigma_j \sigma_i\rangle \,.

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

P_{ij} = \tfrac{1}{2}(\vec{\sigma}_i\cdot\vec{\sigma}_j + 1)\,.

Its eigenvalues are therefore^[5] 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.

SU(2)

The group SU(2) is the Lie group of unitary 2×2 matrices with unit determinant; its Lie algebra is the set of all 2×2 anti-Hermitian matrices with trace 0. Direct calculation, as above, shows that the Lie algebra $\mathfrak{su}_2$ is the 3-dimensional real algebra spanned by the set ${iσ j$ }. In compact notation,

\mathfrak{su}(2) = \operatorname{span} \{ i \sigma_1, i \sigma_2 , i \sigma_3 \}.

As a result, each $iσ j$ can be seen as an infinitesimal generator of SU(2). The elements of SU(2) are exponentials of linear combinations of these three generators, and multiply as indicated above in discussing the Pauli vector. Although this suffices to generate SU(2), it is not a proper representation of $su(2)$ , as the Pauli eigenvalues are scaled unconventionally. The conventional normalization is $λ =$ 1/2, so that

\mathfrak{su}(2) = \operatorname{span} \left\{\frac{i \sigma_1}{2}, \frac{i \sigma_2}{2}, \frac{i \sigma_3}{2} \right\}.

As SU(2) is a compact group, its Cartan decomposition is trivial.

SO(3)

The Lie algebra $su (2)$ is isomorphic to the Lie algebra $so (3)$ , 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 $su (2)$ and $so (3)$ 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

Main article: versor

The real linear span of ${I, iσ 1, iσ 2, iσ 3}$ is isomorphic to the real algebra of quaternions $ℍ$ . The isomorphism from $ℍ$ to this set is given by the following map (notice the reversed signs for the Pauli matrices):

1 \mapsto I, \quad i \mapsto - i \sigma_1, \quad j \mapsto - i \sigma_2, \quad k \mapsto - i \sigma_3.

Alternatively, the isomorphism can be achieved by a map using the Pauli matrices in reversed order,^[6]

1 \mapsto I, \quad i \mapsto i \sigma_3, \quad j \mapsto i \sigma_2, \quad k \mapsto i \sigma_1.

As the quaternions of unit norm is group-isomorphic to $SU(2)$ , this gives yet another way of describing $SU(2)$ via the Pauli matrices. The two-to-one homomorphism from $SU(2)$ to $SO(3)$ can also be explicitly given in terms of the Pauli matrices in this formulation.

Quaternions form a division algebra—every non-zero element has an inverse—whereas Pauli matrices do not. For a quaternionic version of the algebra generated by Pauli matrices see biquaternions, which is a venerable algebra of eight real dimensions.

Physics

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 ½ 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 ½. 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 ½ particles is that they must be rotated by an angle of 4 $π$ 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 $S$ ², they are actually represented by orthogonal vectors in the two dimensional complex Hilbert space.

For a spin ½ particle, the spin operator is given by $J = ħ / 2 σ$ , 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 algebra. 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.

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.

Remarks

↑ The Pauli vector is a formal device. It may be thought of as an element of $M 2 (ℂ) \otimes ℝ 3$ , where the tensor product space is endowed with a mapping $\cdot: ℝ 3 \times M 2 (ℂ) \otimes ℝ 3 \to M 2 (ℂ)$ .
↑ N.B. The relation among $a, b, c, n, m, k$ derived here in the $2 \times 2$ representation holds for all representations of $SU(2)$ , being a group identity.

Notes

↑ "Pauli matrices". Planetmath website. 28 March 2008. Retrieved 28 May 2013.
↑ See the spinor map.
↑ Nielsen, Michael A.; Chuang, Isaac L. (2000). Quantum Computation and Quantum Information. Cambridge, UK: Cambridge University Press. ISBN 978-0-521-63235-5. OCLC 43641333.
↑ cf. J W Gibbs (1884). Elements of Vector Analysis, New Haven, 1884, p. 67
↑ Explicitly, in the convention of "right-space matrices into elements of left-space matrices", it is $\quad \left({\begin{smallmatrix}1&0&0&0\\0&0&1&0\\0&1&0&0\\0&0&0&1\end{smallmatrix}}\right)~.$
↑ Nakahara, Mikio (2003). Geometry, topology, and physics (2nd ed.). CRC Press. ISBN 978-0-7503-0606-5 , pp. xxii.
↑ Curtright, T L; Fairlie, D B; Zachos, C K (2014). "A compact formula for rotations as spin matrix polynomials". SIGMA. 10: 084. arXiv:1402.3541. Bibcode:2014SIGMA..10..084C. doi:10.3842/SIGMA.2014.084.

References

Liboff, Richard L. (2002). Introductory Quantum Mechanics. Addison-Wesley. ISBN 0-8053-8714-5.
Schiff, Leonard I. (1968). Quantum Mechanics. McGraw-Hill. ISBN 978-0070552876.
Leonhardt, Ulf (2010). Essential Quantum Optics. Cambridge University Press. ISBN 0-521-14505-8.

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