3D rotation group

Template:Short description In mechanics and geometry, the 3D rotation group, often denoted SO(3), is the group of all rotations about the origin of three-dimensional Euclidean space <math>\R^3</math> under the operation of composition.<ref>Jacobson (2009), p. 34, Ex. 14.</ref>

By definition, a rotation about the origin is a transformation that preserves the origin, Euclidean distance (so it is an isometry), and orientation (i.e., handedness of space). Composing two rotations results in another rotation, every rotation has a unique inverse rotation, and the identity map satisfies the definition of a rotation. Owing to the above properties (along composite rotations' associative property), the set of all rotations is a group under composition.

Every non-trivial rotation is determined by its axis of rotation (a line through the origin) and its angle of rotation. Rotations are not commutative (for example, rotating R 90° in the x-y plane followed by S 90° in the y-z plane is not the same as S followed by R), making the 3D rotation group a nonabelian group. Moreover, the rotation group has a natural structure as a manifold for which the group operations are smoothly differentiable, so it is in fact a Lie group. It is compact and has dimension 3.

Rotations are linear transformations of <math>\R^3</math> and can therefore be represented by matrices once a basis of <math>\R^3</math> has been chosen. Specifically, if we choose an orthonormal basis of <math>\R^3</math>, every rotation is described by an orthogonal 3 × 3 matrix (i.e., a 3 × 3 matrix with real entries which, when multiplied by its transpose, results in the identity matrix) with determinant 1. The group SO(3) can therefore be identified with the group of these matrices under matrix multiplication. These matrices are known as "special orthogonal matrices", explaining the notation SO(3).

The group SO(3) is used to describe the possible rotational symmetries of an object, as well as the possible orientations of an object in space. Its representations are important in physics, where they give rise to the elementary particles of integer spin.

Length and angle

Besides just preserving length, rotations also preserve the angles between vectors. This follows from the fact that the standard dot product between two vectors u and v can be written purely in terms of length (see the law of cosines): <math display="block">\mathbf{u} \cdot \mathbf{v} = \frac{1}{2} \left(\|\mathbf{u} + \mathbf{v}\|^2 - \|\mathbf{u}\|^2 - \|\mathbf{v}\|^2\right).</math>

It follows that every length-preserving linear transformation in <math>\R^3</math> preserves the dot product, and thus the angle between vectors. Rotations are often defined as linear transformations that preserve the inner product on <math>\R^3</math>, which is equivalent to requiring them to preserve length. See classical group for a treatment of this more general approach, where Template:Math appears as a special case.

Orthogonal and rotation matrices

{{#invoke:Labelled list hatnote|labelledList|Main article|Main articles|Main page|Main pages}}

Every rotation maps an orthonormal basis of <math>\R^3</math> to another orthonormal basis. Like any linear transformation of finite-dimensional vector spaces, a rotation can always be represented by a matrix. Let Template:Math be a given rotation. With respect to the standard basis Template:Math of <math>\R^3</math> the columns of Template:Math are given by Template:Math. Since the standard basis is orthonormal, and since Template:Math preserves angles and length, the columns of Template:Math form another orthonormal basis. This orthonormality condition can be expressed in the form

<math>R^\mathsf{T}R = RR^\mathsf{T} = I,</math>

where Template:Math denotes the transpose of Template:Math and Template:Mvar is the Template:Math identity matrix. Matrices for which this property holds are called orthogonal matrices. The group of all Template:Math orthogonal matrices is denoted Template:Math, and consists of all proper and improper rotations.

In addition to preserving length, proper rotations must also preserve orientation. A matrix will preserve or reverse orientation according to whether the determinant of the matrix is positive or negative. For an orthogonal matrix Template:Math, note that Template:Math implies Template:Math, so that Template:Math. The subgroup of orthogonal matrices with determinant Template:Math is called the special orthogonal group, denoted Template:Math.

Thus every rotation can be represented uniquely by an orthogonal matrix with unit determinant. Moreover, since composition of rotations corresponds to matrix multiplication, the rotation group is isomorphic to the special orthogonal group Template:Math.

Improper rotations correspond to orthogonal matrices with determinant Template:Math, and they do not form a group because the product of two improper rotations is a proper rotation.

Group structure

The rotation group is a group under function composition (or equivalently the product of linear transformations). It is a subgroup of the general linear group consisting of all invertible linear transformations of the real 3-space <math>\R^3</math>.<ref>n × n real matrices are identical to linear transformations of <math>\R^n</math> expressed in its standard basis.</ref>

Furthermore, the rotation group is nonabelian. That is, the order in which rotations are composed makes a difference. For example, a quarter turn around the positive x-axis followed by a quarter turn around the positive y-axis is a different rotation than the one obtained by first rotating around y and then x.

The orthogonal group, consisting of all proper and improper rotations, is generated by reflections. Every proper rotation is the composition of two reflections, a special case of the Cartan–Dieudonné theorem.

Complete classification of finite subgroups

The finite subgroups of <math>\mathrm{SO}(3)</math> are completely classified.<ref name="coxeter">Template:Cite book</ref>

Every finite subgroup is isomorphic to either an element of one of two countably infinite families of planar isometries: the cyclic groups <math>C_n</math> or the dihedral groups <math>D_{2n}</math>, or to one of three other groups: the tetrahedral group <math>\cong A_4</math>, the octahedral group <math>\cong S_4</math>, or the icosahedral group <math>\cong A_5</math>.

Axis of rotation

{{#invoke:Labelled list hatnote|labelledList|Main article|Main articles|Main page|Main pages}} Every nontrivial proper rotation in 3 dimensions fixes a unique 1-dimensional linear subspace of <math>\R^3</math> which is called the axis of rotation (this is Euler's rotation theorem). Each such rotation acts as an ordinary 2-dimensional rotation in the plane orthogonal to this axis. Since every 2-dimensional rotation can be represented by an angle φ, an arbitrary 3-dimensional rotation can be specified by an axis of rotation together with an angle of rotation about this axis. (Technically, one needs to specify an orientation for the axis and whether the rotation is taken to be clockwise or counterclockwise with respect to this orientation).

For example, counterclockwise rotation about the positive z-axis by angle φ is given by

<math>R_z(\phi) = \begin{bmatrix}\cos\phi & -\sin\phi & 0 \\ \sin\phi & \cos\phi & 0 \\ 0 & 0 & 1\end{bmatrix}.</math>

Given a unit vector n in <math>\R^3</math> and an angle φ, let R(φ, n) represent a counterclockwise rotation about the axis through n (with orientation determined by n). Then

• R(0, n) is the identity transformation for any n
• R(φ, n) = R(−φ, −n)
• R(Template:Pi + φ, n) = R(Template:Pi − φ, −n).

Using these properties one can show that any rotation can be represented by a unique angle φ in the range 0 ≤ φ ≤ Template:Pi and a unit vector n such that

• n is arbitrary if φ = 0
• n is unique if 0 < φ < Template:Pi
• n is unique up to a sign if φ = Template:Pi (that is, the rotations R(Template:Pi, ±n) are identical).

In the next section, this representation of rotations is used to identify SO(3) topologically with three-dimensional real projective space.

Topology

{{#invoke:Labelled list hatnote|labelledList|Main article|Main articles|Main page|Main pages}} The Lie group SO(3) is diffeomorphic to the real projective space <math>\mathbb{P}^3(\R).</math><ref>Template:Harvnb Proposition 1.17</ref>

Consider the solid ball in <math>\R^3</math> of radius Template:Pi (that is, all points of <math>\R^3</math> of distance Template:Pi or less from the origin). Given the above, for every point in this ball there is a rotation, with axis through the point and the origin, and rotation angle equal to the distance of the point from the origin. The identity rotation corresponds to the point at the center of the ball. Rotations through an angle Template:Theta between 0 and Template:Pi (not including either) are on the same axis at the same distance. Rotation through angles between 0 and −Template:Pi correspond to the point on the same axis and distance from the origin but on the opposite side of the origin. The one remaining issue is that the two rotations through Template:Pi and through −Template:Pi are the same. So we identify (or "glue together") antipodal points on the surface of the ball. After this identification, we arrive at a topological space homeomorphic to the rotation group.

Indeed, the ball with antipodal surface points identified is a smooth manifold, and this manifold is diffeomorphic to the rotation group. It is also diffeomorphic to the real 3-dimensional projective space <math>\mathbb{P}^3(\R),</math> so the latter can also serve as a topological model for the rotation group.

These identifications illustrate that SO(3) is connected but not simply connected. As to the latter, in the ball with antipodal surface points identified, consider the path running from the "north pole" straight through the interior down to the south pole. This is a closed loop, since the north pole and the south pole are identified. This loop cannot be shrunk to a point, since no matter how it is deformed, the start and end point have to remain antipodal, or else the loop will "break open". In terms of rotations, this loop represents a continuous sequence of rotations about the z-axis starting (by example) at the identity (center of the ball), through the south pole, jumping to the north pole and ending again at the identity rotation (i.e., a series of rotation through an angle φ where φ runs from 0 to [[turn (geometry)|2Template:Pi]]).

Surprisingly, running through the path twice, i.e., running from the north pole down to the south pole, jumping back to the north pole (using the fact that north and south poles are identified), and then again running from the north pole down to the south pole, so that φ runs from 0 to 4Template:Pi, gives a closed loop which can be shrunk to a single point: first move the paths continuously to the ball's surface, still connecting north pole to south pole twice. The second path can then be mirrored over to the antipodal side without changing the path at all. Now we have an ordinary closed loop on the surface of the ball, connecting the north pole to itself along a great circle. This circle can be shrunk to the north pole without problems. The plate trick and similar tricks demonstrate this practically.

The same argument can be performed in general, and it shows that the fundamental group of SO(3) is the cyclic group of order 2 (a fundamental group with two elements). In physics applications, the non-triviality (more than one element) of the fundamental group allows for the existence of objects known as spinors, and is an important tool in the development of the spin–statistics theorem.

The universal cover of SO(3) is a Lie group called Spin(3). The group Spin(3) is isomorphic to the special unitary group SU(2); it is also diffeomorphic to the unit 3-sphere S³ and can be understood as the group of versors (quaternions with absolute value 1). The connection between quaternions and rotations, commonly exploited in computer graphics, is explained in quaternions and spatial rotations. The map from S³ onto SO(3) that identifies antipodal points of S³ is a surjective homomorphism of Lie groups, with kernel {±1}. Topologically, this map is a two-to-one covering map. (See the plate trick.)

Connection between SO(3) and SU(2)

In this section, we give two different constructions of a two-to-one and surjective homomorphism of SU(2) onto SO(3).

Using quaternions of unit norm

{{#invoke:Labelled list hatnote|labelledList|Main article|Main articles|Main page|Main pages}} The group Template:Math is isomorphic to the quaternions of unit norm via a map given by<ref>Template:Harvnb p. 95.</ref> <math display="block">q = a\mathbf{1} + b\mathbf{i} + c\mathbf{j} + d\mathbf{k} = \alpha + \beta \mathbf{j} \leftrightarrow \begin{bmatrix}\alpha & \beta \\ -\overline\beta & \overline \alpha\end{bmatrix} = U</math> restricted to <math display="inline">a^2+ b^2 + c^2 + d^2 = |\alpha|^2 +|\beta|^2 = 1</math> where <math display="inline"> q \in \mathbb{H}</math>, <math display="inline">a, b, c, d \in \R</math>, <math display="inline"> U \in \operatorname{SU}(2)</math>, and <math>\alpha = a+bi \in\mathbb{C}</math>, <math>\beta = c+di \in \mathbb{C}</math>.

Let us now identify <math>\R^3</math> with the span of <math>\mathbf{i},\mathbf{j},\mathbf{k}</math>. One can then verify that if <math>v</math> is in <math>\R^3</math> and <math>q</math> is a unit quaternion, then <math display="block">qvq^{-1}\in \R^3.</math>

Furthermore, the map <math>v\mapsto qvq^{-1}</math> is a rotation of <math>\R^3.</math> Moreover, <math>(-q)v(-q)^{-1}</math> is the same as <math>qvq^{-1}</math>. This means that there is a Template:Math homomorphism from quaternions of unit norm to the 3D rotation group Template:Math.

One can work this homomorphism out explicitly: the unit quaternion, Template:Mvar, with <math display="block">\begin{align}

q &= w + x\mathbf{i} + y\mathbf{j} + z\mathbf{k} , \\
1 &= w^2 + x^2 + y^2 + z^2 ,

\end{align}</math> is mapped to the rotation matrix <math display="block"> Q = \begin{bmatrix}

1 - 2 y^2 - 2 z^2 & 2 x y - 2 z w & 2 x z + 2 y w \\
2 x y + 2 z w & 1 - 2 x^2 - 2 z^2 & 2 y z - 2 x w \\
2 x z - 2 y w & 2 y z + 2 x w & 1 - 2 x^2 - 2 y^2

\end{bmatrix}. </math>

This is a rotation around the vector Template:Math by an angle Template:Math, where Template:Math and Template:Math. The proper sign for Template:Math is implied, once the signs of the axis components are fixed. The Template:Nowrap is apparent since both Template:Math and Template:Math map to the same Template:Math.

Using Möbius transformations

File:Stereoprojnegone.svg

Stereographic projection from the sphere of radius Template:Math from the north pole Template:Math onto the plane Template:Mvar given by Template:Math coordinatized by Template:Math, here shown in cross section.

The general reference for this section is Template:Harvtxt. The points Template:Math on the sphere

<math>\mathbf{S} = \left \{(x,y,z)\in\R^3: x^2 +y^2 +z^2 = \frac{1}{4} \right \}</math>

can, barring the north pole Template:Math, be put into one-to-one bijection with points Template:Math on the plane Template:Math defined by Template:Math, see figure. The map Template:Math is called stereographic projection.

Let the coordinates on Template:Mvar be Template:Math. The line Template:Math passing through Template:Math and Template:Math can be parametrized as

<math>L(t) = N + t(N - P) = \left(0,0,\frac{1}{2}\right) + t \left ( \left(0,0,\frac{1}{2}\right) - (x, y, z) \right ), \quad t\in \R.</math>

Demanding that the Template:Nowrap of <math>L(t_0)</math> equals Template:Math, one finds

<math>t_0 = \frac1{z-\frac12}.</math>

We have <math>L(t_0)=(\xi,\eta,-1/2).</math> Hence the map

<math>\begin{cases} S:\mathbf{S} \to M \\ P = (x,y,z) \longmapsto P'= (\xi, \eta) = \left(\frac{x}{\frac{1}{2} - z}, \frac{y}{\frac{1}{2} - z}\right) \equiv \zeta = \xi + i\eta \end{cases}</math>

where, for later convenience, the plane Template:Math is identified with the complex plane <math>\Complex.</math>

For the inverse, write Template:Math as

<math>L = N + s(P'-N) = \left(0,0,\frac{1}{2}\right) + s\left( \left(\xi, \eta, -\frac{1}{2}\right) - \left(0,0,\frac{1}{2}\right)\right),</math>

and demand Template:Math to find Template:Math and thus

<math>\begin{cases} S^{-1}:M \to \mathbf{S} \\ P'= (\xi, \eta) \longmapsto P = (x,y,z) = \left(\frac{\xi}{1 + \xi^2 + \eta^2}, \frac{\eta}{1 + \xi^2 + \eta^2}, \frac{-1 + \xi^2 + \eta^2}{2 + 2\xi^2 + 2\eta^2}\right) \end{cases}</math>

If Template:Math is a rotation, then it will take points on Template:Math to points on Template:Math by its standard action Template:Math on the embedding space <math>\R^3.</math> By composing this action with Template:Math one obtains a transformation Template:Math of Template:Mvar,

<math>\zeta=P' \longmapsto P \longmapsto \Pi_s(g)P = gP \longmapsto S(gP) \equiv \Pi_u(g)\zeta = \zeta'.</math>

Thus Template:Math is a transformation of <math>\Complex</math> associated to the transformation Template:Math of <math>\R^3</math>.

It turns out that Template:Math represented in this way by Template:Math can be expressed as a matrix Template:Math (where the notation is recycled to use the same name for the matrix as for the transformation of <math>\Complex</math> it represents). To identify this matrix, consider first a rotation Template:Math about the Template:Nowrap through an angle Template:Mvar,

<math>\begin{align}

x' &= x\cos \phi - y \sin \phi,\\ y' &= x\sin \phi + y \cos \phi,\\ z' &= z. \end{align}</math>

Hence

<math>\zeta' = \frac{x' + iy'}{\frac{1}{2} - z'} = \frac{e^{i\phi}(x + iy)}{\frac{1}{2} - z} = e^{i\phi}\zeta = \frac{e^{\frac{i\phi}{2}} \zeta + 0 }{0 \zeta + e^{-\frac{i\phi}{2}}},</math>

which, unsurprisingly, is a rotation in the complex plane. In an analogous way, if Template:Math is a rotation about the Template:Nowrap through an angle Template:Mvar, then

<math>w' = e^{i\theta}w, \quad w = \frac{y + iz}{\frac{1}{2} - x},</math>

which, after a little algebra, becomes

<math>\zeta' = \frac{\cos \frac{\theta}{2}\zeta +i\sin \frac{\theta}{2} }{i \sin\frac{\theta}{2}\zeta + \cos\frac{\theta}{2}}.</math>

These two rotations, <math>g_{\phi}, g_{\theta},</math> thus correspond to bilinear transforms of Template:Math, namely, they are examples of Möbius transformations.

A general Möbius transformation is given by

<math>\zeta' = \frac{\alpha \zeta + \beta}{\gamma \zeta + \delta}, \quad \alpha\delta - \beta\gamma \ne 0.</math>

The rotations, <math>g_{\phi}, g_{\theta}</math> generate all of Template:Math and the composition rules of the Möbius transformations show that any composition of <math>g_{\phi}, g_{\theta}</math> translates to the corresponding composition of Möbius transformations. The Möbius transformations can be represented by matrices

<math>\begin{pmatrix}\alpha & \beta\\ \gamma & \delta\end{pmatrix}, \qquad \alpha\delta - \beta\gamma = 1,</math>

since a common factor of Template:Math cancels.

For the same reason, the matrix is not uniquely defined since multiplication by Template:Math has no effect on either the determinant or the Möbius transformation. The composition law of Möbius transformations follow that of the corresponding matrices. The conclusion is that each Möbius transformation corresponds to two matrices Template:Math.

Using this correspondence one may write

<math>\begin{align}

\Pi_u(g_\phi) &= \Pi_u\left[\begin{pmatrix} \cos \phi & -\sin \phi & 0\\ \sin \phi & \cos \phi & 0\\ 0 & 0 & 1 \end{pmatrix}\right] = \pm \begin{pmatrix} e^{i\frac{\phi}{2}} & 0\\ 0 & e^{-i\frac{\phi}{2}} \end{pmatrix},\\ \Pi_u(g_\theta) &= \Pi_u\left[\begin{pmatrix} 1 & 0 & 0\\ 0 & \cos \theta & -\sin \theta\\ 0 & \sin \theta & \cos \theta \end{pmatrix}\right] = \pm \begin{pmatrix} \cos\frac{\theta}{2} & i\sin\frac{\theta}{2}\\ i\sin\frac{\theta}{2} & \cos\frac{\theta}{2} \end{pmatrix}. \end{align}</math>

These matrices are unitary and thus Template:Math. In terms of Euler angles<ref group="nb">This is effected by first applying a rotation <math>g_{\theta}</math> through Template:Mvar about the Template:Nowrap to take the Template:Nowrap to the line Template:Math, the intersection between the planes Template:Math and Template:Math, the latter being the rotated Template:Nowrap. Then rotate with <math>g_{\theta}</math> through Template:Mvar about Template:Math to obtain the new Template:Nowrap from the old one, and finally rotate by <math>g_{\psi}</math> through an angle Template:Mvar about the new Template:Nowrap, where Template:Mvar is the angle between Template:Mvar and the new Template:Nowrap. In the equation, <math>g_{\theta}</math> and <math>g_{\psi}</math> are expressed in a temporary rotated basis at each step, which is seen from their simple form. To transform these back to the original basis, observe that <math>\mathbf{g}_{\theta} = g_{\phi}g_{\theta}g_{\phi}^{-1}.</math> Here boldface means that the rotation is expressed in the original basis. Likewise,

<math>\mathbf{g}_{\psi} = g_{\phi}g_{\theta}g_{\phi}^{-1} g_{\phi} g_{\psi} \left [ g_{\phi}g_{\theta}g_{\phi}^{-1} g_{\phi} \right ]^{-1}.</math>

Thus

<math>\mathbf{g}_{\psi}\mathbf{g}_{\theta}\mathbf{g}_{\phi} = g_{\phi}g_{\theta}g_{\phi}^{-1} g_{\phi}g_{\psi} \left [g_{\phi} g_{\theta} g_{\phi}^{-1} g_{\phi} \right ]^{-1} * g_{\phi}g_{\theta}g_{\phi}^{-1}* g_{\phi} = g_{\phi}g_{\theta}g_{\psi}.</math></ref> one finds for a general rotation

one has<ref>These expressions were, in fact, seminal in the development of quantum mechanics in the 1930s, cf. Ch III,  § 16, B.L. van der Waerden, 1932/1932</ref>

Template:NumBlk & 0\\ 0 & e^{-i\frac{\phi}{2}} \end{pmatrix} \begin{pmatrix} \cos\frac{\theta}{2} & i\sin\frac{\theta}{2}\\ i\sin\frac{\theta}{2} & \cos\frac{\theta}{2} \end{pmatrix} \begin{pmatrix} e^{i\frac{\psi}{2}} & 0\\ 0 & e^{-i\frac{\psi}{2}} \end{pmatrix}\\ &= \pm \begin{pmatrix} \cos\frac{\theta}{2}e^{i\frac{\phi + \psi}{2}} & i\sin\frac{\theta}{2}e^{i\frac{\phi - \psi}{2}}\\ i\sin\frac{\theta}{2}e^{-i\frac{\phi - \psi}{2}} & \cos\frac{\theta}{2}e^{-i\frac{\phi + \psi}{2}} \end{pmatrix}. \end{align}</math>|Template:EquationRef}}

For the converse, consider a general matrix

<math>\pm\Pi_u(g_{\alpha,\beta}) = \pm\begin{pmatrix} \alpha & \beta\\ -\overline{\beta} & \overline{\alpha} \end{pmatrix} \in \operatorname{SU}(2).</math>

Make the substitutions

<math>\begin{align}

  \cos\frac{\theta}{2} &= |\alpha|,    &  \sin\frac{\theta}{2} &= |\beta|,    & (0 \le \theta \le \pi),\\
 \frac{\phi + \psi}{2} &= \arg \alpha, & \frac{\psi - \phi}{2} &= \arg \beta. &

\end{align}</math>

With the substitutions, Template:Math assumes the form of the right hand side (RHS) of (Template:EquationNote), which corresponds under Template:Math to a matrix on the form of the RHS of (Template:EquationNote) with the same Template:Math. In terms of the complex parameters Template:Math,

<math>g_{\alpha,\beta} = \begin{pmatrix}

  \frac{1}{2}\left( \alpha^2 - \beta^2 + \overline{\alpha^2} - \overline{\beta^2}\right) &
  \frac{i}{2}\left(-\alpha^2 - \beta^2 + \overline{\alpha^2} + \overline{\beta^2}\right) &
                   -\alpha\beta - \overline{\alpha}\overline{\beta}\\

  \frac{i}{2}\left(\alpha^2 - \beta^2 - \overline{\alpha^2} + \overline{\beta^2}\right) &
  \frac{1}{2}\left(\alpha^2 + \beta^2 + \overline{\alpha^2} + \overline{\beta^2}\right) &
                 -i\left(+\alpha\beta - \overline{\alpha}\overline{\beta}\right)\\

          \alpha\overline{\beta}  + \overline{\alpha}\beta &
  i\left(-\alpha\overline{\beta}  + \overline{\alpha}\beta\right) &
          \alpha\overline{\alpha} - \beta\overline{\beta}

\end{pmatrix}.</math>

To verify this, substitute for Template:Math the elements of the matrix on the RHS of (Template:EquationNote). After some manipulation, the matrix assumes the form of the RHS of (Template:EquationNote).

It is clear from the explicit form in terms of Euler angles that the map

<math> \begin{cases}

p:\operatorname{SU}(2) \to \operatorname{SO}(3)\\ \pm \Pi_u(g_{\alpha \beta}) \mapsto g_{\alpha \beta} \end{cases}</math>

just described is a smooth, Template:Math and surjective group homomorphism. It is hence an explicit description of the universal covering space of Template:Math from the universal covering group Template:Math.

Lie algebra

Associated with every Lie group is its Lie algebra, a linear space of the same dimension as the Lie group, closed under a bilinear alternating product called the Lie bracket. The Lie algebra of Template:Math is denoted by <math>\mathfrak{so}(3)</math> and consists of all skew-symmetric Template:Math matrices.<ref>Template:Harvnb Proposition 3.24</ref> This may be seen by differentiating the orthogonality condition, Template:Math.<ref group="nb">For an alternative derivation of <math>\mathfrak{so}(3)</math>, see Classical group.</ref> The Lie bracket of two elements of <math>\mathfrak{so}(3)</math> is, as for the Lie algebra of every matrix group, given by the matrix commutator, Template:Math, which is again a skew-symmetric matrix. The Lie algebra bracket captures the essence of the Lie group product in a sense made precise by the Baker–Campbell–Hausdorff formula.

The elements of <math>\mathfrak{so}(3)</math> are the "infinitesimal generators" of rotations, i.e., they are the elements of the tangent space of the manifold SO(3) at the identity element. If <math>R(\phi, \boldsymbol{n})</math> denotes a counterclockwise rotation with angle φ about the axis specified by the unit vector <math>\boldsymbol{n},</math> then

<math>\forall \boldsymbol{u} \in \R^3: \qquad \left. \frac{\operatorname{d}}{\operatorname{d}\phi} \right|_{\phi=0} R(\phi,\boldsymbol{n}) \boldsymbol{u} = \boldsymbol{n} \times \boldsymbol{u}.</math>

This can be used to show that the Lie algebra <math>\mathfrak{so}(3)</math> (with commutator) is isomorphic to the Lie algebra <math>\R^3</math> (with cross product). Under this isomorphism, an Euler vector <math>\boldsymbol{\omega}\in\R^3</math> corresponds to the linear map <math>\widetilde{\boldsymbol{\omega}}</math> defined by <math>\widetilde{\boldsymbol{\omega}}(\boldsymbol{u}) = \boldsymbol{\omega}\times\boldsymbol{u}.</math>

In more detail, most often a suitable basis for <math>\mathfrak{so}(3)</math> as a Template:Nowrap vector space is

<math>

\boldsymbol{L}_x = \begin{bmatrix}0&0&0\\0&0&-1\\0&1&0\end{bmatrix}, \quad \boldsymbol{L}_y = \begin{bmatrix}0&0&1\\0&0&0\\-1&0&0\end{bmatrix}, \quad \boldsymbol{L}_z = \begin{bmatrix}0&-1&0\\1&0&0\\0&0&0\end{bmatrix}. </math>

The commutation relations of these basis elements are,

<math>

[\boldsymbol{L}_x, \boldsymbol{L}_y] = \boldsymbol{L}_z, \quad [\boldsymbol{L}_z, \boldsymbol{L}_x] = \boldsymbol{L}_y, \quad [\boldsymbol{L}_y, \boldsymbol{L}_z] = \boldsymbol{L}_x </math>

which agree with the relations of the three standard unit vectors of <math>\R^3</math> under the cross product.

As announced above, one can identify any matrix in this Lie algebra with an Euler vector <math>\boldsymbol{\omega} = (x,y,z) \in \R^3,</math><ref>Template:Harvnb</ref>

<math>\widehat{\boldsymbol{\omega}} =\boldsymbol{\omega}\cdot \boldsymbol{L} = x \boldsymbol{L}_x + y \boldsymbol{L}_y + z \boldsymbol{L}_z =\begin{bmatrix}0&-z&y\\z&0&-x\\-y&x&0\end{bmatrix} \in \mathfrak{so}(3).</math>

This identification is sometimes called the hat-map.<ref name="Engø 2001">Template:Harvnb</ref> Under this identification, the <math>\mathfrak{so}(3)</math> bracket corresponds in <math>\R^3</math> to the cross product,

<math>\left [\widehat{\boldsymbol{u}},\widehat{\boldsymbol{v}} \right ] = \widehat{\boldsymbol{u} \times \boldsymbol{v}}.</math>

The matrix identified with a vector <math>\boldsymbol{u}</math> has the property that

<math>\widehat{\boldsymbol{u}}\boldsymbol{v} = \boldsymbol{u} \times \boldsymbol{v},</math>

where the left-hand side we have ordinary matrix multiplication. This implies <math>\boldsymbol{u}</math> is in the null space of the skew-symmetric matrix with which it is identified, because <math>\boldsymbol{u} \times \boldsymbol{u} = \boldsymbol{0}.</math>

A note on Lie algebras

{{#invoke:Labelled list hatnote|labelledList|Main article|Main articles|Main page|Main pages}} Template:See also

In Lie algebra representations, the group SO(3) is compact and simple of rank 1, and so it has a single independent Casimir element, a quadratic invariant function of the three generators which commutes with all of them. The Killing form for the rotation group is just the Kronecker delta, and so this Casimir invariant is simply the sum of the squares of the generators, <math>\boldsymbol{J}_x, \boldsymbol{J}_y, \boldsymbol{J}_z,</math> of the algebra

<math>

[\boldsymbol{J}_x, \boldsymbol{J}_y] = \boldsymbol{J}_z, \quad [\boldsymbol{J}_z, \boldsymbol{J}_x] = \boldsymbol{J}_y, \quad [\boldsymbol{J}_y, \boldsymbol{J}_z] = \boldsymbol{J}_x. </math> That is, the Casimir invariant is given by

<math>\boldsymbol{J}^2\equiv \boldsymbol{J}\cdot \boldsymbol{J} =\boldsymbol{J}_x^2+\boldsymbol{J}_y^2+\boldsymbol{J}_z^2 \propto \boldsymbol{I}.</math>

For unitary irreducible representations Template:Mvar, the eigenvalues of this invariant are real and discrete, and characterize each representation, which is finite dimensional, of dimensionality <math>2j+1</math>. That is, the eigenvalues of this Casimir operator are

<math>\boldsymbol{J}^2=- j(j+1) \boldsymbol{I}_{2j+1},</math>

where Template:Mvar is integer or half-integer, and referred to as the spin or angular momentum.

So, the 3 × 3 generators L displayed above act on the triplet (spin 1) representation, while the 2 × 2 generators below, t, act on the doublet (spin-1/2) representation. By taking Kronecker products of Template:Math with itself repeatedly, one may construct all higher irreducible representations Template:Mvar. That is, the resulting generators for higher spin systems in three spatial dimensions, for arbitrarily large Template:Mvar, can be calculated using these spin operators and ladder operators.

For every unitary irreducible representations Template:Mvar there is an equivalent one, Template:Math. All infinite-dimensional irreducible representations must be non-unitary, since the group is compact.

In quantum mechanics, the Casimir invariant is the "angular-momentum-squared" operator; integer values of spin Template:Mvar characterize bosonic representations, while half-integer values fermionic representations. The antihermitian matrices used above are utilized as spin operators, after they are multiplied by Template:Mvar, so they are now hermitian (like the Pauli matrices). Thus, in this language,

<math>

[\boldsymbol{J}_x, \boldsymbol{J}_y] = i\boldsymbol{J}_z, \quad [\boldsymbol{J}_z, \boldsymbol{J}_x] = i\boldsymbol{J}_y, \quad [\boldsymbol{J}_y, \boldsymbol{J}_z] = i\boldsymbol{J}_x. </math> and hence

<math>\boldsymbol{J}^2= j(j+1) \boldsymbol{I}_{2j+1}.</math>

Explicit expressions for these Template:Mvar are,

<math>\begin{align}

\left (\boldsymbol{J}_z^{(j)}\right )_{ba} &= (j+1-a)\delta_{b,a}\\ \left (\boldsymbol{J}_x^{(j)}\right )_{ba} &=\frac{1}{2} \left (\delta_{b,a+1}+\delta_{b+1,a} \right ) \sqrt{(j+1)(a+b-1)-ab}\\ \left (\boldsymbol{J}_y^{(j)}\right )_{ba} &=\frac{1}{2i} \left (\delta_{b,a+1}-\delta_{b+1,a} \right ) \sqrt{(j+1)(a+b-1)-ab}\\ \end{align}</math> where Template:Mvar is arbitrary and <math>1 \le a, b \le 2j+1</math>.

For example, the resulting spin matrices for spin 1 (<math>j = 1</math>) are

<math>\begin{align}

\boldsymbol{J}_x &= \frac{1}{\sqrt{2}}

\begin{pmatrix}
0 &1 &0\\
1 &0 &1\\
0 &1 &0
\end{pmatrix} \\

\boldsymbol{J}_y &= \frac{1}{\sqrt{2}}

\begin{pmatrix}
0 &-i &0\\
i &0 &-i\\
0 &i &0
\end{pmatrix} \\

\boldsymbol{J}_z &=

\begin{pmatrix}
1 &0 &0\\
0 &0 &0\\
0 &0 &-1
\end{pmatrix}

\end{align}</math>

Note, however, how these are in an equivalent, but different basis, the spherical basis, than the above Template:MvarL in the Cartesian basis.<ref group="nb">Specifically, <math>\boldsymbol{U} \boldsymbol{J}_{\alpha}\boldsymbol{U}^\dagger=i\boldsymbol{L}_\alpha</math> for

<math>\boldsymbol{U}= \left(

\begin{array}{ccc}

-\frac{i}{\sqrt{2}} & 0 & \frac{i}{\sqrt{2}} \\
\frac{1}{\sqrt{2}} & 0 & \frac{1}{\sqrt{2}} \\
0 & i & 0 \\

\end{array} \right).</math></ref>

For higher spins, such as spin Template:Sfrac (<math>j=\tfrac{3}{2}</math>):

<math>\begin{align}

\boldsymbol{J}_x &= \frac{1}{2}

\begin{pmatrix}
0 &\sqrt{3} &0 &0\\
\sqrt{3} &0 &2 &0\\
0 &2 &0 &\sqrt{3}\\
0 &0 &\sqrt{3} &0
\end{pmatrix} \\

\boldsymbol{J}_y &= \frac{1}{2}

\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} \\

\boldsymbol{J}_z &=\frac{1}{2}

\begin{pmatrix}
3 &0 &0 &0\\
0 &1 &0 &0\\
0 &0 &-1 &0\\
0 &0 &0 &-3
\end{pmatrix}.

\end{align}</math>

For spin Template:Sfrac (<math>j = \tfrac{5}{2}</math>),

<math>\begin{align}

\boldsymbol{J}_x &= \frac{1}{2}

\begin{pmatrix}
0 &\sqrt{5} &0 &0 &0 &0 \\
\sqrt{5} &0 &2\sqrt{2} &0 &0 &0 \\
0 &2\sqrt{2} &0 &3 &0 &0 \\
0 &0 &3 &0 &2\sqrt{2} &0 \\
0 &0 &0 &2\sqrt{2} &0 &\sqrt{5} \\
0 &0 &0 &0 &\sqrt{5} &0
\end{pmatrix} \\

\boldsymbol{J}_y &= \frac{1}{2}

\begin{pmatrix}
0 &-i\sqrt{5} &0 &0 &0 &0 \\
i\sqrt{5} &0 &-2i\sqrt{2} &0 &0 &0 \\
0 &2i\sqrt{2} &0 &-3i &0 &0 \\
0 &0 &3i &0 &-2i\sqrt{2} &0 \\
0 &0 &0 &2i\sqrt{2} &0 &-i\sqrt{5} \\
0 &0 &0 &0 &i\sqrt{5} &0
\end{pmatrix} \\

\boldsymbol{J}_z &= \frac{1}{2}

\begin{pmatrix}
5 &0 &0 &0 &0 &0 \\
0 &3 &0 &0 &0 &0 \\
0 &0 &1 &0 &0 &0 \\
0 &0 &0 &-1 &0 &0 \\
0 &0 &0 &0 &-3 &0 \\
0 &0 &0 &0 &0 &-5
\end{pmatrix}.

\end{align}</math>

{{#invoke:Labelled list hatnote|labelledList|Main article|Main articles|Main page|Main pages}}

Isomorphism with 𝖘𝖚(2)

The Lie algebras <math>\mathfrak{so}(3)</math> and <math>\mathfrak{su}(2)</math> are isomorphic. One basis for <math>\mathfrak{su}(2)</math> is given by<ref>Template:Harvnb Example 3.27</ref>

<math>\boldsymbol{t}_1 = \frac{1}{2}\begin{bmatrix}0 & -i\\ -i & 0\end{bmatrix}, \quad \boldsymbol{t}_2 = \frac{1}{2} \begin{bmatrix}0 & -1\\ 1 & 0\end{bmatrix}, \quad \boldsymbol{t}_3 = \frac{1}{2}\begin{bmatrix}-i & 0\\ 0 & i\end{bmatrix}.</math>

These are related to the Pauli matrices by

<math>\boldsymbol{t}_i \longleftrightarrow \frac{1}{2i} \sigma_i.</math>

The Pauli matrices abide by the physicists' convention for Lie algebras. In that convention, Lie algebra elements are multiplied by Template:Mvar, the exponential map (below) is defined with an extra factor of Template:Mvar in the exponent and the structure constants remain the same, but the definition of them acquires a factor of Template:Mvar. Likewise, commutation relations acquire a factor of Template:Mvar. The commutation relations for the <math>\boldsymbol{t}_i</math> are

<math>[\boldsymbol{t}_i, \boldsymbol{t}_j] = \varepsilon_{ijk}\boldsymbol{t}_k,</math>

where Template:Math is the totally anti-symmetric symbol with Template:Math. The isomorphism between <math>\mathfrak{so}(3)</math> and <math>\mathfrak{su}(2)</math> can be set up in several ways. For later convenience, <math>\mathfrak{so}(3)</math> and <math>\mathfrak{su}(2)</math> are identified by mapping

<math>\boldsymbol{L}_x \longleftrightarrow \boldsymbol{t}_1, \quad \boldsymbol{L}_y \longleftrightarrow \boldsymbol{t}_2, \quad \boldsymbol{L}_z \longleftrightarrow \boldsymbol{t}_3,</math>

and extending by linearity.

Exponential map

The exponential map for Template:Math, is, since Template:Math is a matrix Lie group, defined using the standard matrix exponential series,

<math>\begin{cases}

\exp : \mathfrak{so}(3) \to \operatorname{SO}(3) \\ A \mapsto e^A = \sum_{k=0}^\infty \frac{1}{k!} A^k

= I + A + \tfrac{1}{2} A^2 + \cdots.

\end{cases}</math>

For any skew-symmetric matrix Template:Math, Template:Math is always in Template:Math. The proof uses the elementary properties of the matrix exponential

<math>\left(e^A\right)^\textsf{T} e^A = e^{A^\textsf{T}} e^A = e^{A^\textsf{T} + A} = e^{-A + A} = e^{A - A} = e^A \left(e^A\right)^\textsf{T} = e^0 = I.</math>

since the matrices Template:Math and Template:Math commute, this can be easily proven with the skew-symmetric matrix condition. This is not enough to show that Template:Math is the corresponding Lie algebra for Template:Math, and shall be proven separately.

The level of difficulty of proof depends on how a matrix group Lie algebra is defined. Template:Harvtxt defines the Lie algebra as the set of matrices

<math>\left\{A \in \operatorname{M}(n, \R) \left| e^{tA} \in \operatorname{SO}(3) \forall t\right.\right\},</math>

in which case it is trivial. Template:Harvtxt uses for a definition derivatives of smooth curve segments in Template:Math through the identity taken at the identity, in which case it is harder.<ref>See Template:Harvnb, theorem 3, section 2.2.</ref>

For a fixed Template:Math, Template:Math is a one-parameter subgroup along a geodesic in Template:Math. That this gives a one-parameter subgroup follows directly from properties of the exponential map.<ref>Template:Harvnb Section 1.1.</ref>

The exponential map provides a diffeomorphism between a neighborhood of the origin in the Template:Math and a neighborhood of the identity in the Template:Math.<ref>Template:Harvnb Theorem 2.27.</ref> For a proof, see Closed subgroup theorem.

The exponential map is surjective. This follows from the fact that every Template:Math, since every rotation leaves an axis fixed (Euler's rotation theorem), and is conjugate to a block diagonal matrix of the form

<math>D = \begin{pmatrix}\cos \theta & -\sin \theta & 0\\ \sin \theta & \cos \theta & 0\\ 0 & 0 & 1\end{pmatrix} = e^{\theta L_z},</math>

such that Template:Math, and that

<math>Be^{\theta L_z}B^{-1} = e^{B\theta L_zB^{-1}},</math>

together with the fact that Template:Math is closed under the adjoint action of Template:Math, meaning that Template:Math.

Thus, e.g., it is easy to check the popular identity

<math>e^{-\pi L_x/2} e^{\theta L_z} e^{\pi L_x/2} = e^{\theta L_y}.</math>

As shown above, every element Template:Math is associated with a vector Template:Math, where Template:Math is a unit magnitude vector. Since Template:Math is in the null space of Template:Mvar, if one now rotates to a new basis, through some other orthogonal matrix Template:Math, with Template:Math as the Template:Mvar axis, the final column and row of the rotation matrix in the new basis will be zero.

Thus, we know in advance from the formula for the exponential that Template:Math must leave Template:Math fixed. It is mathematically impossible to supply a straightforward formula for such a basis as a function of Template:Math, because its existence would violate the hairy ball theorem; but direct exponentiation is possible, and yields

<math>\begin{align}

\exp(\tilde{\boldsymbol{\omega}})
  &= \exp(\theta(\boldsymbol{u\cdot L}))
   = \exp\left(\theta \begin{bmatrix} 0 & -z & y \\ z & 0 & -x \\ -y & x & 0 \end{bmatrix}\right)\\[4pt]
  &= \boldsymbol{I} + 2cs(\boldsymbol{u\cdot L}) + 2s^2 (\boldsymbol{u \cdot L})^2 \\[4pt]
  &= \begin{bmatrix}
       2 \left(x^2 - 1\right) s^2 + 1 & 2 x y s^2 - 2 z c s & 2 x z s^2 + 2 y c s \\
       2 x y s^2 + 2 z c s & 2 \left(y^2 - 1\right) s^2 + 1 & 2 y z s^2 - 2 x c s \\
       2 x z s^2 - 2 y c s & 2 y z s^2 + 2 x c s & 2 \left(z^2 - 1\right) s^2 + 1
     \end{bmatrix},

\end{align}</math>

where <math display="inline">c = \cos\frac{\theta}{2}</math> and <math display="inline">s = \sin\frac{\theta}{2}</math>. This is recognized as a matrix for a rotation around axis Template:Math by the angle Template:Mvar: cf. Rodrigues' rotation formula.

Logarithm map

Given Template:Math, let <math>A = \tfrac{1}{2} \left(R - R^\mathrm{T}\right)</math> denote the antisymmetric part and let <math display="inline">\|A\| = \sqrt{-\frac{1}{2}\operatorname{Tr}\left(A^2\right)}.</math> Then, the logarithm of Template:Mvar is given by<ref name="Engø 2001"/>

<math>\log R = \frac{\sin^{-1}\|A\|}{\|A\|}A.</math>

This is manifest by inspection of the mixed symmetry form of Rodrigues' formula,

<math>e^X = I + \frac{\sin \theta}{\theta}X + 2\frac{\sin^2\frac{\theta}{2}}{\theta^2}X^2, \quad \theta = \|X\|,</math>

where the first and last term on the right-hand side are symmetric.

Uniform random sampling

<math>SO(3)</math> is doubly covered by the group of unit quaternions, which is isomorphic to the 3-sphere. Since the Haar measure on the unit quaternions is just the 3-area measure in 4 dimensions, the Haar measure on <math>SO(3)</math> is just the pushforward of the 3-area measure.

Consequently, generating a uniformly random rotation in <math>\R^3</math> is equivalent to generating a uniformly random point on the 3-sphere. This can be accomplished by the following<math display="block">(\sqrt{1-u_1}\sin(2\pi u_2), \sqrt{1-u_1}\cos(2\pi u_2), \sqrt{u_1}\sin(2\pi u_3), \sqrt{u_1}\cos(2\pi u_3))</math>

where <math>u_1, u_2, u_3</math> are uniformly random samples of <math>[0, 1]</math>.<ref>Template:Citation</ref>

Baker–Campbell–Hausdorff formula

{{#invoke:Labelled list hatnote|labelledList|Main article|Main articles|Main page|Main pages}} Suppose Template:Mvar and Template:Mvar in the Lie algebra are given. Their exponentials, Template:Math and Template:Math, are rotation matrices, which can be multiplied. Since the exponential map is a surjection, for some Template:Mvar in the Lie algebra, Template:Math, and one may tentatively write

<math> Z = C(X, Y),</math>

for Template:Mvar some expression in Template:Math and Template:Math. When Template:Math and Template:Math commute, then Template:Math, mimicking the behavior of complex exponentiation.

The general case is given by the more elaborate BCH formula, a series expansion of nested Lie brackets.<ref>Template:Harvnb; Template:Harvnb</ref> For matrices, the Lie bracket is the same operation as the commutator, which monitors lack of commutativity in multiplication. This general expansion unfolds as follows,<ref group="nb">For a full proof, see Derivative of the exponential map. Issues of convergence of this series to the correct element of the Lie algebra are here swept under the carpet. Convergence is guaranteed when <math>\|X\| + \|Y\| < \log 2 </math> and <math>\|Z\| < \log 2.</math> The series may still converge even if these conditions are not fulfilled. A solution always exists since Template:Math is onto in the cases under consideration.</ref>

<math>Z = C(X, Y) = X + Y + \frac{1}{2} [X, Y] + \tfrac{1}{12} [X, [X, Y]] - \frac{1}{12} [Y, [X, Y]] + \cdots.</math>

The infinite expansion in the BCH formula for Template:Math reduces to a compact form,

<math>Z = \alpha X + \beta Y + \gamma[X, Y],</math>

for suitable trigonometric function coefficients Template:Math. Template:Hidden begin The Template:Math are given by

<math>\alpha = \phi \cot\left(\frac{\phi}{2}\right) \gamma, \qquad \beta = \theta \cot\left(\frac{\theta}{2}\right)\gamma, \qquad \gamma = \frac{\sin^{-1}d}{d}\frac{c}{\theta \phi},</math>

where

<math>\begin{align}

 c &= \frac{1}{2}\sin\theta\sin\phi - 2\sin^2\frac{\theta}{2}\sin^2\frac{\phi}{2}\cos(\angle(u, v)),\quad a = c \cot\left(\frac{\phi}{2}\right), \quad b = c \cot\left(\frac{\theta}{2}\right), \\
 d &= \sqrt{a^2 + b^2 + 2ab\cos(\angle(u, v)) + c^2 \sin^2(\angle(u, v))},

\end{align}</math>

for

<math>\theta = \|X\|,\quad \phi = \|Y\|,\quad \angle(u, v) = \cos^{-1}\frac{\langle X, Y\rangle}{\|X\|\|Y\|}.</math>

The inner product is the Hilbert–Schmidt inner product and the norm is the associated norm. Under the hat-isomorphism,

<math>\langle u, v\rangle = \frac{1}{2}\operatorname{Tr}X^\mathrm{T}Y,</math>

which explains the factors for Template:Mvar and Template:Mvar. This drops out in the expression for the angle. Template:See also Template:Hidden end

It is worthwhile to write this composite rotation generator as

<math>\alpha X + \beta Y + \gamma[X, Y]\underset{\mathfrak{so}(3)}{=} X + Y + \frac{1}{2} [X, Y] + \frac{1}{12} [X, [X, Y]] - \frac{1}{12} [Y, [X, Y]] + \cdots,</math>

to emphasize that this is a Lie algebra identity.

The above identity holds for all faithful representations of Template:Math. The kernel of a Lie algebra homomorphism is an ideal, but Template:Math, being simple, has no nontrivial ideals and all nontrivial representations are hence faithful. It holds in particular in the doublet or spinor representation. The same explicit formula thus follows in a simpler way through Pauli matrices, cf. the 2×2 derivation for SU(2).

Template:Hidden begin The Pauli vector version of the same BCH formula is the somewhat simpler group composition law of SU(2),

<math>

 e^{i a'\left(\hat{u} \cdot \vec{\sigma}\right)}e^{i b'\left(\hat{v} \cdot \vec{\sigma}\right)} =
 \exp\left(
   \frac{c'}{\sin c'} \sin a' \sin b' \left(\left(i\cot b'\hat{u} + i \cot a' \hat{v}\right)\cdot\vec{\sigma} +
   \frac{1}{2} \left[i \hat{u} \cdot \vec{\sigma}, i \hat{v} \cdot \vec{\sigma}\right]\right)
 \right),

</math>

where

<math>\cos c' = \cos a' \cos b' - \hat{u} \cdot\hat{v} \sin a' \sin b',</math>

the spherical law of cosines. (Note Template:Math are angles, not the Template:Math above.)

This is manifestly of the same format as above,

<math>Z = \alpha' X + \beta' Y + \gamma' [X, Y],</math>

with

<math>X = i a'\hat{u} \cdot \mathbf{\sigma}, \quad Y = ib'\hat{v} \cdot \mathbf{\sigma} \in \mathfrak{su}(2),</math>

so that

<math>\begin{align}

 \alpha' &= \frac{c'}{\sin c'}\frac{\sin a'}{a'}\cos b' \\ 
  \beta' &= \frac{c'}{\sin c'}\frac{\sin b'}{b'}\cos a' \\ 
 \gamma' &= \frac{1}{2}\frac{c'}{\sin c'}\frac{\sin a'}{a'}\frac{\sin b'}{b'}.

\end{align}</math>

For uniform normalization of the generators in the Lie algebra involved, express the Pauli matrices in terms of Template:Mvar-matrices, Template:Math, so that

<math>a' \mapsto -\frac{\theta}{2}, \quad b' \mapsto - \frac{\phi}{2}.</math>

To verify then these are the same coefficients as above, compute the ratios of the coefficients,

<math>\begin{align}

 \frac{\alpha'}{\gamma'} &= \theta\cot\frac{\theta}{2} &= \frac{\alpha}{\gamma}\\
  \frac{\beta'}{\gamma'} &= \phi\cot\frac{\phi}{2} &= \frac{\beta}{\gamma}.

\end{align}</math> Finally, Template:Math given the identity Template:Math. Template:Hidden end

For the general Template:Math case, one might use Ref.<ref>Template:Harvnb Group elements of SU(2) are expressed in closed form as finite polynomials of the Lie algebra generators, for all definite spin representations of the rotation group.</ref>

Template:Hidden begin The quaternion formulation of the composition of two rotations R_B and R_A also yields directly the rotation axis and angle of the composite rotation R_C = R_BR_A.

Let the quaternion associated with a spatial rotation R is constructed from its rotation axis S and the rotation angle φ this axis. The associated quaternion is given by,

<math>S = \cos\frac{\phi}{2} + \sin\frac{\phi}{2} \mathbf{S}.</math>

Then the composition of the rotation R_R with R_A is the rotation R_C = R_BR_A with rotation axis and angle defined by the product of the quaternions

<math>A = \cos\frac{\alpha}{2} + \sin\frac{\alpha}{2}\mathbf{A}\quad\text{ and }\quad B = \cos\frac{\beta}{2} + \sin\frac{\beta}{2}\mathbf{B},</math>

that is

<math>

 C = \cos\frac{\gamma}{2} + \sin\frac{\gamma}{2}\mathbf{C} =
 \left(\cos\frac{\beta}{2} + \sin\frac{\beta}{2}\mathbf{B}\right)\left(\cos\frac{\alpha}{2} + \sin\frac{\alpha}{2}\mathbf{A}\right).</math>

Expand this product to obtain

<math>

 \cos\frac{\gamma}{2} + \sin\frac{\gamma}{2} \mathbf{C} =
 \left(
   \cos\frac{\beta}{2}\cos\frac{\alpha}{2} -
   \sin\frac{\beta}{2}\sin\frac{\alpha}{2} \mathbf{B}\cdot \mathbf{A}
 \right) + \left(
   \sin\frac{\beta}{2}\cos\frac{\alpha}{2} \mathbf{B} +
   \sin\frac{\alpha}{2}\cos\frac{\beta}{2} \mathbf{A} +
   \sin\frac{\beta}{2}\sin\frac{\alpha}{2} \mathbf{B} \times \mathbf{A}
 \right).

</math>

Divide both sides of this equation by the identity, which is the law of cosines on a sphere,

<math>\cos\frac{\gamma}{2} = \cos\frac{\beta}{2}\cos\frac{\alpha}{2} - \sin\frac{\beta}{2}\sin\frac{\alpha}{2} \mathbf{B}\cdot \mathbf{A},</math>

and compute

<math>\tan\frac{\gamma}{2} \mathbf{C} = \frac{\tan\frac{\beta}{2}\mathbf{B} + \tan\frac{\alpha}{2} \mathbf{A} + \tan\frac{\beta}{2}\tan\frac{\alpha}{2} \mathbf{B} \times \mathbf{A}}{1 - \tan\frac{\beta}{2}\tan\frac{\alpha}{2} \mathbf{B} \cdot \mathbf{A}}.</math>

This is Rodrigues' formula for the axis of a composite rotation defined in terms of the axes of the two rotations. He derived this formula in 1840 (see page 408).<ref>Rodrigues, O. (1840), Des lois géométriques qui régissent les déplacements d'un système solide dans l'espace, et la variation des coordonnées provenant de ses déplacements con- sidérés indépendamment des causes qui peuvent les produire, Journal de Mathématiques Pures et Appliquées de Liouville 5, 380–440.</ref>

The three rotation axes A, B, and C form a spherical triangle and the dihedral angles between the planes formed by the sides of this triangle are defined by the rotation angles.

Realizations of rotations

{{#invoke:Labelled list hatnote|labelledList|Main article|Main articles|Main page|Main pages}} Template:See also

We have seen that there are a variety of ways to represent rotations:

• as orthogonal matrices with determinant 1,
• by axis and rotation angle
• in quaternion algebra with versors and the map 3-sphere S³ → SO(3) (see quaternions and spatial rotations)
• in geometric algebra as a rotor
• as a sequence of three rotations about three fixed axes; see Euler angles.

Spherical harmonics

{{#invoke:Labelled list hatnote|labelledList|Main article|Main articles|Main page|Main pages}} Template:See also

The group Template:Math of three-dimensional Euclidean rotations has an infinite-dimensional representation on the Hilbert space

<math>L^2\left(\mathbf{S}^2\right) = \operatorname{span} \left\{ Y^\ell_m, \ell \in \N^+, -\ell \leq m \leq \ell \right\}, </math>

where <math>Y^\ell_m</math> are spherical harmonics. Its elements are square integrable complex-valued functions<ref group=nb>The elements of Template:Math are actually equivalence classes of functions. two functions are declared equivalent if they differ merely on a set of measure zero. The integral is the Lebesgue integral in order to obtain a complete inner product space.</ref> on the sphere. The inner product on this space is given by

If Template:Mvar is an arbitrary square integrable function defined on the unit sphere Template:Math, then it can be expressed as<ref name="Gelfand_M_S">Template:Harvnb</ref>

where the expansion coefficients are given by

The Lorentz group action restricts to that of Template:Math and is expressed as

This action is unitary, meaning that

The Template:Math can be obtained from the Template:Math of above using Clebsch–Gordan decomposition, but they are more easily directly expressed as an exponential of an odd-dimensional Template:Math-representation (the 3-dimensional one is exactly Template:Math).<ref>In Quantum Mechanics – non-relativistic theory by Landau and Lifshitz the lowest order Template:Math are calculated analytically.</ref><ref>Template:Harvnb A formula for Template:Math valid for all ℓ is given.</ref> In this case the space Template:Math decomposes neatly into an infinite direct sum of irreducible odd finite-dimensional representations Template:Math according to<ref>Template:Harvnb Section 4.3.5.</ref>

This is characteristic of infinite-dimensional unitary representations of Template:Math. If Template:Mvar is an infinite-dimensional unitary representation on a separable<ref group=nb>A Hilbert space is separable if and only if it has a countable basis. All separable Hilbert spaces are isomorphic.</ref> Hilbert space, then it decomposes as a direct sum of finite-dimensional unitary representations.<ref name=Gelfand_M_S/> Such a representation is thus never irreducible. All irreducible finite-dimensional representations Template:Math can be made unitary by an appropriate choice of inner product,<ref name=Gelfand_M_S/>

<math>\langle f, g\rangle_U \equiv \int_{\operatorname{SO}(3)} \langle\Pi(R)f, \Pi(R)g\rangle \, dg = \frac{1}{8\pi^2} \int_0^{2\pi} \int_0^\pi \int_0^{2\pi} \langle \Pi(R)f, \Pi(R)g\rangle \sin \theta \, d\phi \, d\theta \, d\psi, \quad f,g \in V,</math>

where the integral is the unique invariant integral over Template:Math normalized to Template:Math, here expressed using the Euler angles parametrization. The inner product inside the integral is any inner product on Template:Math.

Generalizations

The rotation group generalizes quite naturally to n-dimensional Euclidean space, <math>\R^n</math> with its standard Euclidean structure. The group of all proper and improper rotations in n dimensions is called the orthogonal group O(n), and the subgroup of proper rotations is called the special orthogonal group SO(n), which is a Lie group of dimension Template:Nowrap.

In special relativity, one works in a 4-dimensional vector space, known as Minkowski space rather than 3-dimensional Euclidean space. Unlike Euclidean space, Minkowski space has an inner product with an indefinite signature. However, one can still define generalized rotations which preserve this inner product. Such generalized rotations are known as Lorentz transformations and the group of all such transformations is called the Lorentz group.

The rotation group SO(3) can be described as a subgroup of E⁺(3), the Euclidean group of direct isometries of Euclidean <math>\R^3.</math> This larger group is the group of all motions of a rigid body: each of these is a combination of a rotation about an arbitrary axis and a translation, or put differently, a combination of an element of SO(3) and an arbitrary translation.

In general, the rotation group of an object is the symmetry group within the group of direct isometries; in other words, the intersection of the full symmetry group and the group of direct isometries. For chiral objects it is the same as the full symmetry group.

See also

• Orthogonal group
• Angular momentum
• Coordinate rotations
• Charts on SO(3)
• Representations of SO(3)
• Euler angles
• Rodrigues' rotation formula
• Infinitesimal rotation
• Pin group
• Quaternions and spatial rotations
• Rigid body
• Spherical harmonics
• Plane of rotation
• Lie group
• Pauli matrix
• Plate trick
• Three-dimensional rotation operator

Bibliography

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