Pauli matrices

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The Pauli matrices are a set of 2 × 2 complex Hermitian and unitary matrices. Usually indicated by the Greek letter 'sigma' (σ), they are occasionally denoted with a 'tau' (τ) when used in connection with isospin symmetries. They are:

$\sigma_1 = \sigma_x = \begin{pmatrix} 0&1\\ 1&0 \end{pmatrix}$

$\sigma_2 = \sigma_y = \begin{pmatrix} 0&-i\\ i&0 \end{pmatrix}$

$\sigma_3 = \sigma_z = \begin{pmatrix} 1&0\\ 0&-1 \end{pmatrix}$

The name refers to Wolfgang Pauli.

1 Algebraic properties
- 1.1 Commutation relations
2 SU(2)
3 Physics
- 3.1 Quantum mechanics
- 3.2 Quantum information
4 See also
5 References

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

where I is the identity matrix.

The determinants and traces of the Pauli matrices are:

$\begin{matrix} \det (\sigma_i) &=& -1 & \\[1ex] \operatorname{Tr} (\sigma_i) &=& 0 & \quad \hbox{for}\ i = 1, 2, 3 \end{matrix}$

From above we can deduce that the eigenvalues of each σ_i are ±1.

Together with the identity matrix I (which is sometimes written as σ₀), the Pauli matrices form an orthogonal basis, in the sense of Hilbert-Schmidt, for the real Hilbert space of 2 × 2 complex Hermitian matrices, or the complex Hilbert space of all 2 × 2 matrices.

The Pauli matrices obey the following commutation and anticommutation relations:

$\begin{matrix} [\sigma_i, \sigma_j] &=& 2 i\,\varepsilon_{i j k}\,\sigma_k \\[1ex] \{\sigma_i, \sigma_j\} &=& 2 \delta_{i j} \cdot I \end{matrix}$

where $\varepsilon_{ijk}$ is the Levi-Civita symbol, $δ i j$ is the Kronecker delta, and I is the identity matrix.

The above two relations can be summarized as:

$\sigma_i \sigma_j = \delta_{ij} \cdot I + i \varepsilon_{ijk} \sigma_k \,$ .

For example,

$\begin{matrix} \sigma_1\sigma_2 &=& i\sigma_3,\\ \sigma_2\sigma_3 &=& i\sigma_1,\\ \sigma_2\sigma_1 &=& -i\sigma_3,\\ \sigma_1\sigma_1 &=& I.\\ \end{matrix}$

The pauli vector is defined by

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

and the summary equation for the commutation relations can be used to prove

$(\vec{a} \cdot \vec{\sigma})(\vec{b} \cdot \vec{\sigma}) = \vec{a} \cdot \vec{b} + i \vec{\sigma} \cdot ( \vec{a} \times \vec{b} ) \quad \quad \quad \quad (1) \,$

(as long as the vectors a and b commute with the pauli matrices)

as well as

$e^{i (\vec{a} \cdot \vec{\sigma})} = \cos{a} + i (\hat{n} \cdot \vec{\sigma}) \sin{a} \quad \quad \quad \quad \quad \quad (2) \,$

for $\vec{a} = a \hat{n}$ .

Proof of (1)

$(\vec{a} \cdot \vec{\sigma})(\vec{b} \cdot \vec{\sigma}) \,$	$= a_i \sigma_i b_j \sigma_j \,$
	$= a_i b_j \sigma_i \sigma_j \,$
	$= a_i b_j \left( \delta_{ij} \cdot I+ i \varepsilon_{ijk} \sigma_k \right) \,$
	$= a_i b_j \delta_{ij} \cdot I+ i \sigma_k \varepsilon_{ijk} a_i b_j \,$
	$= \vec{a} \cdot \vec{b} + i \vec{\sigma} \cdot ( \vec{a} \times \vec{b} )\,$

Proof of (2)

First notice that for even powers

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

but for odd powers

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

Combine these two facts with the knowledge of the relation of the exponential to sine and cosine:

$e^{ix} \,$	$= \sum_{n=0}^\infty{\frac{i^n x^n}{n!}} \,$
	$= \sum_{n=0}^\infty{\frac{(-1)^n x^{2n}}{2n!}} + i\sum_{n=0}^\infty{\frac{(-1)^n x^{2n+1}}{(2n+1)!}} \,$

Which, when we use $x = a (\hat{n} \cdot \vec{\sigma}) \,$ gives us

$= \sum_{n=0}^\infty{\frac{(-1)^n (a\hat{n}\cdot \vec{\sigma})^{2n}}{2n!}} + i\sum_{n=0}^\infty{\frac{(-1)^n (a\hat{n}\cdot \vec{\sigma})^{2n+1}}{(2n+1)!}} \,$

$= \sum_{n=0}^\infty{\frac{(-1)^n a^{2n}}{2n!}} + i (\hat{n}\cdot \vec{\sigma}) \sum_{n=0}^\infty{\frac{(-1)^n a^{2n+1}}{(2n+1)!}} \,$

The sum on the left is cosine, and the sum on the right is sine so finally,

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

The matrix group SU(2) is a Lie group, and its Lie algebra is the set of the anti-Hermitian 2×2 matrices with trace 0. Direct calculation shows that the Lie algebra su(2) is the 3 dimensional real algebra spanned by the set {i σ_j}. In symbols,

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

As a result, i σ_js can be seen as infinitesimal generators of SU(2).

This relationship between the Pauli matrices and SU(2) can be explored further, as can be seen from the following simple example. We can write

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

We put

$\; \mathfrak{k} = \operatorname{span} \{i \sigma_3\},$

and

$\; \mathfrak{p} = \operatorname{span} \{ i \sigma_1, i \sigma_2\}$

Using the algebraic identities listed in the previous section, it can be verified that $\mathfrak{k}$ and $\mathfrak{p}$ form a Cartan pair of the Lie algebra su(2). Furthermore,

$\; \mathfrak{a} = \operatorname{span} \{ i \sigma_2\}$

is a maximal abelian subalgebra of $\mathfrak{p}$ . Now, a version of Cartan decomposition states that any element U in the Lie group SU(2) can be expressed in the form

$U = e^{k_1} e^a e^{k_2}\,\!$ where $k_1, k_2 \in \mathfrak{k}$ and $a \in \mathfrak{a}.$

In other words, any unitary U of determinant 1 is of the form

$U = e^{i \alpha \sigma_3} e^{i \beta \sigma_2} e^{i \gamma \sigma_3}\,\!$

for some real numbers α, β, and γ.

Extending to unitary matrices gives that any unitary 2 × 2 U is of the form

$U = e^{i \delta} e^{i \alpha \sigma_3} e^{i \beta \sigma_2} e^{i \gamma \sigma_3}\,\!$

where the additional parameter δ is also real.

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 $i σ j$ 's are a realization (and, in fact, the lowest-dimensional realization) of infinitesimal rotations in three-dimensional space. It might be of interest here to note that even though their infinitesimal generators 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 homomorphism from SU(2) to SO(3).

Consider the real linear span S of {I, σ₁ σ₂, σ₂ σ₃, σ₃ σ₁}. S is isomorphic to the real algebra of quaternions H. The isomorphism from H to S is given by

$1 \simeq 1, i \simeq \sigma_1 \sigma_2, j \simeq \sigma_3 \sigma_1, k \simeq \sigma_2 \sigma_3.$

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 - there always is an inverse - whereas Pauli matrices do not.

In quantum mechanics, each Pauli matrix represents an observable describing the spin of a spin ½ particle in the three spatial directions. Also, as an immediate consequence of the Cartan decomposition mentioned above, $i σ j$ are the generators of rotation acting on non-relativistic particles with spin ½. The state of the particles are represented as two-component spinors. 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 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 $\mathbf{J} =\frac\hbar2\boldsymbol{\sigma}$ . The Pauli matrices can be generalized to describe higher spin systems in three spatial dimensions. The spin matrices for spin 1 and spin ³⁄₂ are given below:

j=1:

$J_x = \frac\hbar\sqrt{2} \begin{pmatrix} 0&1&0\\ 1&0&1\\ 0&1&0 \end{pmatrix}$

$J_y = \frac\hbar\sqrt{2} \begin{pmatrix} 0&-i&0\\ i&0&-i\\ 0&i&0 \end{pmatrix}$

$J_z = \hbar \begin{pmatrix} 1&0&0\\ 0&0&0\\ 0&0&-1 \end{pmatrix}$

j=³⁄₂:

$J_x = \frac\hbar2 \begin{pmatrix} 0&\sqrt{3}&0&0\\ \sqrt{3}&0&2&0\\ 0&2&0&\sqrt{3}\\ 0&0&\sqrt{3}&0 \end{pmatrix}$

$J_y = \frac\hbar2 \begin{pmatrix} 0&-i\sqrt{3}&0&0\\ i\sqrt{3}&0&-2i&0\\ 0&2i&0&-i\sqrt{3}\\ 0&0&i\sqrt{3}&0 \end{pmatrix}$

$J_z = \frac\hbar2 \begin{pmatrix} 3&0&0&0\\ 0&1&0&0\\ 0&0&-1&0\\ 0&0&0&-3 \end{pmatrix}$

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.

The fact that any 2 × 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 × 2 mixed states (2 × 2 positive semidefinite matrices with trace 1). This can be seen by simply first writing a Hermitian matrix as a real linear combination of {σ₀, σ₁, σ₂, σ₃} then impose the positive semidefinite and trace 1 assumptions.

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.

Liboff, Richard L. (2002). Introductory Quantum Mechanics. Addison-Wesley. ISBN 0-8053-8714-5.

Schiff, Leonard I. (1968). Quantum Mechanics. McGraw-Hill. ISBN 007-Y85643-5.

Retrieved from "http://en.wikipedia.org/wiki/Pauli_matrices"

Categories: Lie groups | Matrices | Rotational symmetry

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Pauli matrices

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