# Rotation group SO(3)

{{#invoke:Hatnote|hatnote}}Template:Main other

In mechanics and geometry, the **3D rotation group** is the group of all rotations about the origin of three-dimensional Euclidean space **R**^{3} under the operation of composition.^{[1]} 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). A distance-preserving transformation which reverses orientation is an improper rotation, that is a reflection or, in the general position, a rotoreflection. The origin in Euclidean space establishes a one-to-one correspondence between points and their coordinate vectors. Rotations about the origin can be thought of as magnitude-preserving linear transformations of Euclidean 3-dimensional vectors (whose vector space is also denoted as **R**^{3}).

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 with the associative property, which rotations obey), the set of all rotations is a group under composition. Moreover, the rotation group has a natural manifold structure for which the group operations are smooth; so it is in fact a Lie group. The rotation group is often denoted **SO(3)** (or, less ambiguously, SO(3, **R**)) for reasons explained below.

## 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:

It follows that any length-preserving transformation in **R**^{3} preserves the dot product, and thus the angle between vectors. Rotations are often defined as linear transformations that preserve the inner product on **R**^{3}, which is equivalent to requiring them to preserve length. See classical group for a treatment of this more general approach, where SO(3) appears as a special case.

## Orthogonal and rotation matrices

{{#invoke:main|main}}

Every rotation maps an orthonormal basis of **R**^{3} to another orthonormal basis. Like any linear transformation of finite-dimensional vector spaces, a rotation can always be represented by a matrix. Let *R* be a given rotation. With respect to the standard basis **e**_{1}, **e**_{2}, **e**_{3} of **R**^{3} the columns of *R* are given by (*R***e**_{1}, *R***e**_{2}, *R***e**_{3}). Since the standard basis is orthonormal, and since *R* preserves angles and length, the columns of *R* form another orthonormal basis. This orthonormality condition can be expressed in the form

where *R*^{Template:Sans-serif} denotes the transpose of *R* and Template:Mvar is the 3 × 3 identity matrix. Matrices for which this property holds are called orthogonal matrices. The group of all 3 × 3 orthogonal matrices is denoted O(3), 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 *R*, note that det *R*^{Template:Sans-serif} = det *R*^{−1} implies (det *R*)^{2} = 1, so that det *R* = ±1. The subgroup of orthogonal matrices with determinant +1 is called the *special orthogonal group*, denoted SO(3).

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 SO(3).

Improper rotations correspond to orthogonal matrices with determinant −1, 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 **R**^{3}.^{[2]}

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.

## Axis of rotation

{{#invoke:main|main}}
Every nontrivial proper rotation in 3 dimensions fixes a unique 1-dimensional linear subspace of **R**^{3} 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

Given a unit vector **n** in **R**^{3} 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*(π + φ,**n**) =*R*(π − φ, −**n**).

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

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

## Topology

{{#invoke:main|main}}
The Lie group SO(3) is diffeomorphic to the real projective space **RP**^{3}.

Consider the solid ball in **R**^{3} of radius π (that is, all points of **R**^{3} of distance π 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. Rotation through angles between 0 and −π 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 π and through −π 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 **RP**^{3}, 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 you deform the loop, 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 and ending at the identity rotation (i.e. a series of rotation through an angle φ where φ runs from 0 to 2π).

Surprisingly, if you run through the path twice, i.e., run from north pole down to south pole, jump back to the north pole (using the fact that north and south poles are identified), and then again run from north pole down to south pole, so that φ runs from 0 to 4π, you get 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 half of the 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 Balinese 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 cyclic group of order 2. In physics applications, the non-triviality 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 *S*^{3} 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 *S*^{3} onto SO(3) that identifies antipodal points of *S*^{3} is a surjective homomorphism of Lie groups, with kernel {±1}. Topologically, this map is a two-to-one covering map.

## Connection between SO(3) and SU(2)

The general reference for this section is Template:Harvtxt. The points *P* on the sphere **S** = {(*x*, *y*, *z*) ∈ ℝ^{3}: *x*^{2} + *y*^{2} + *z*^{2} = {{ safesubst:#invoke:Unsubst||$B=1/4}}} can, barring the north pole *N*, be put into one-to-one bijection with points *S*(*P*) = *P*´ on the plane *M* defined by *z* = −{{ safesubst:#invoke:Unsubst||$B=1/2}}, see figure. The map *S* is called stereographic projection.

Let the coordinates on Template:Mvar be (*ξ*, *η*). The line *L* passing through *N* and *P* can be written

Demanding that the *z*-coordinate equals −{{ safesubst:#invoke:Unsubst||$B=1/2}}, one finds *t* = {{ safesubst:#invoke:Unsubst||$B=1/*z* − Template:Frac}}, hence

where, for later convenience, the plane *M* is identified with the complex plane ℂ.

For the inverse, write *L* as

and demand *x*^{2} + *y*^{2} + *z*^{2} = {{ safesubst:#invoke:Unsubst||$B=1/4}} to find *s* = {{ safesubst:#invoke:Unsubst||$B=1/1 + *ξ*^{2} + *η*^{2}}} and thus

If *g* ∈ SO(3) is a rotation, then it will take points on **S** to points on **S** by its standard action Π_{s}(*g*) on the embedding space ℝ^{3}. By composing this action with *S* one obtains a transformation *S* ∘ Π_{s}(*g*) ∘ *S*^{−1} of Template:Mvar, *ζ* = *P´* ↦ *P* ↦ Π_{s}(*g*)*P* =*gP* ↦ *S*(*gP*) ≡ Π_{u}(*g*)*ζ* = *ζ´*. Thus Π_{u}(*g*) is a transformation of ℂ associated to the transformation Π_{s}(*g*) of ℝ^{3}.

It turns out that *g* ∈ SO(3) represented in this way by Π_{u}(*g*) can be expressed as a matrix Π_{u}(*g*) ∈ SU(2) (where the notation is recycled to use the same name for the matrix as for the transformation of ℂ it represents). To identify this matrix, consider first a rotation *g*_{φ} about the *z*-axis through an angle Template:Mvar,

Hence

which, unsurprisingly, is a rotation in the complex plane. In an analogous way, if *g*_{θ} is a rotation about the *x*-axis through and angle Template:Mvar, then

which, after a little algebra, becomes

These two rotations, *g*_{φ}, *g*_{θ}, thus correspond to bilinear transforms of ℝ^{2} ≃ ℂ ≃ *M*, namely, they are examples of Möbius transformations.

A general Möbius transformation is given by

The rotations, *g*_{φ}, *g*_{θ} generate all of SO(3) and the composition rules of the Möbius transformations show that any composition of *g*_{φ}, *g*_{θ} translates to the corresponding composition of Möbius transformations. The Möbius transformations can be represented by matrices

since a common factor of *α*, *β*, *γ*, *δ* cancels.

For the same reason, the matrix is *not* uniquely defined since multiplication by −*I* 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 *g*, −*g* ∈ SL(2, ℂ).

Using this correspondence one may write

These matrices are unitary and thus Π_{u}(SO(3)) ⊂ SU(2) ⊂ SL(2, ℂ). In terms of Euler angles^{[nb 1]} one finds for a general rotation
Template:NumBlk
one has^{[3]}
Template:NumBlk

For the converse, consider a general matrix

Make the substitutions

With the substitutions, Π(*g*_{α, β}) assumes the form of the right hand side (RHS) of Template:EquationNote, which corresponds under Π_{u} to a matrix on the form of the RHS of Template:EquationNote with the same *φ*, *θ*, *ψ*. In terms of the complex parameters *α*, *β*,

To verify this, substitute for *α*. *β* 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 *p*:SU(2) → SO(3);Π(±g_{αβ}) ↦ g_{αβ} just described is a smooth, 2:1 and onto group homomorphism. It is hence an explicit description of the universal covering map of SO(3) from the universal covering group SU(2).

### Quaternions of unit norm

SU(2) is isomorphic to the quaternions of unit norm via a map given by

This means that there is a 2:1 homomorphism from quaternions of unit norm to SO(3). Concretely, a unit quaternion, Template:Mvar, with

is mapped to the rotation matrix

This is a rotation around the vector (*x*,*y*,*z*) by an angle 2*θ*, where cos *θ* = w and |sin *θ*| = ||(*x*,*y*,*z*)||. The proper sign for sin *θ* is implied, once the signs of the axis components are fixed. The 2:1-nature is apparent since both *q* and −*q* map to the same *Q*.

## 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 SO(*3*) is denoted by **so**(3)
and consists of all skew-symmetric *3* × *3* matrices. This may be seen by differentiating the orthogonality condition, *A*^{T}*A* = *I*, *A* ∈ SO(3).^{[nb 2]} The Lie bracket of two elements of **so**(3) is, as for the Lie algebra of every matrix group, given by the **matrix commutator**, [*A*_{1}, *A*_{2}] = *A*_{1}*A*_{2} − *A*_{2}*A*_{1}, 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.

A most often suitable basis for **so**(3) as a 3-dimensional vector space is

The commutation relations of these basis elements are,

One can conveniently identify any matrix in this Lie algebra with a vector in ℝ^{3},^{[5]}

This identification is sometimes called the **hat-map**.^{[6]} Under this identification, the **so**(3) bracket corresponds in ℝ^{3} to the cross product,

hence ℝ^{3} is itself a Lie algebra with the Lie bracket being the cross product.
The matrix identified with a vector **u** has the property that

where ordinary matrix multiplication is implied on the left hand side. This implies that **u** is in the null space of the skew-symmetric matrix with which it is identified, because **u** × **u** = 0.

### Isomorphism with su(2)

The Lie algebras **so**(3) and **su**(2) are isomorphic. One basis for **su**(2) is given by

These are related to the Pauli matrices by *t*_{i} ↔ {{ safesubst:#invoke:Unsubst||$B=1/2*i*}}*σ*_{i}. The Pauli matrices abide the physicist 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 *t*_{i} are

where *ε*_{ijk} is the totally anti-symmetric symbol with *ε*_{123} = 1. The isomorphism between **so**(3) and **su**(2) can be set up in several ways. For later convenience, **so**(3) and **su**(2) are identified by mapping

and extending by linearity.

## Exponential map

The exponential map for SO(3), is, since SO(3) is a matrix Lie group, defined using the standard matrix exponential series,

For any skew-symmetric matrix *A* ∈ **so**(3), *e ^{A}* is always in SO(3). 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

*A*∈

*M*

_{n}(ℝ)| e

^{tA}∈ SO(3) ∀

*t*, in which case it is trivial. Template:Harvtxt uses for a definition derivatives of smooth curve segments in SO(3) through the identity taken at the identity, in which case it is harder.

^{[7]}

For a fixed *A* ≠ 0, *e*^{tA}, −∞ < *t* < ∞ is a one-parameter subgroup along a geodesic in SO(3). That this gives a one-parameter subgroup follows directly from properties of the exponential map.^{[8]}

The exponential map provides a diffeomorphism between a neighborhood of the origin in the **so**(3) and a neighborhood of the identity in the SO(3).^{[9]} For a proof, see Closed subgroup theorem.

The exponential map is surjective. This follows from the fact that that every *R* ∈ SO(3), since every rotation leaves an axis fixed (Euler's rotation theorem), and is conjugate to a block diagonal matrix of the form

such that *A* = *BDB*^{−1}, and that

together with the fact that **so**(3) is closed under the adjoint action of SO(3), meaning that *BθL _{z}B*

^{−1}∈

**so**(3).

As shown above, every element *A* ∈ **so**(3) is associated with a vector * ω* =

*θ*

*, where*

**u***= (*

**u***x*,

*y*,

*z*) is a unit magnitude vector. Since

*is in the null space of Template:Mvar, if one now rotates to a new basis, through some other orthogonal matrix*

**u***O*, with

**u**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 exp(*OAO*^{T}) must leave * u* fixed. It is mathematically impossible to supply a straightforward formula for such a basis as a function of

*, because its existence would violate the hairy ball theorem; but direct exponentiation is possible, and yields*

**u**where *c* = cosTemplate:Frac, *s* = sinTemplate:Frac. This is recognized as a matrix for a rotation around axis * u* by the angle Template:Mvar: cf. Rodrigues' rotation formula.

## Logarithm map

Given *R* ∈ SO(3), let

denote the antisymmetric part. Then the logarithm of Template:Mvar is given by^{[10]}

The proof is found by examination of Rodrigues' formula on the mixed form

observing that the first and last term on the right hand side are symmetric.

## Baker–Campbell–Hausdorff formula

{{#invoke:main|main}}
Suppose Template:Mvar and Template:Mvar in the Lie algebra are given. Their exponentials, exp(*X*) and exp(*Y*), are rotation matrices, which can be multiplied. Since the exponential map is a surjection, for some Template:Mvar in the Lie algebra, exp(*Z*) = exp(*X*) exp(*Y*), and one may tentatively write

for Template:Mvar some expression in *X* and *Y*. When exp(*X*) and exp(*Y*) commute, then *Z* = *X* + *Y*, mimicking the behavior of complex exponentiation.

The general case is given by the more elaborate BCH formula, a series expansion of nested Lie brackets.^{[11]} 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,^{[nb 3]}

The infinite expansion in the BCH formula for SO(3) reduces to a compact form,

for suitable trigonometric function coefficients (*α*, *β*, *γ*).
Template:Hidden begin
The (*α*, *β*, *γ*) are given by

where

for

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

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

It is worthwhile to write this composite rotation generator as

to emphasize that this is a *Lie algebra identity*.

The above identity holds for all faithful representations of **so**(3). The kernel of a Lie algebra homomorphism is an ideal, but **so**(3), 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),

where

the spherical law of cosines. (Note * a', b' ,c' * are angles, not the *a,b,c* above.)

This is manifestly of the same format as above,

with

so that

For uniform normalization of the generators in the Lie algebra involved, express the Pauli matrices in terms of Template:Mvar-matrices, * σ* →2

*i*

*, so that*

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

Finally, *γ* = *γ' * given the identity *d* = sin 2*c'*.
Template:Hidden end

For the general *n* × *n* case, one might use Ref.^{[12]}

## Infinitesimal rotations

The matrices in the Lie algebra are not themselves rotations; the skew-symmetric matrices are derivatives. An actual "differential rotation", or *infinitesimal rotation matrix* has the form

where *dθ* is vanishingly small and *A* ∈ SO(3).

These matrices do not satisfy all the same properties as ordinary finite rotation matrices under the usual treatment of infinitesimals .^{[13]} To understand what this means, one considers

First, test the orthogonality condition, *Q ^{T}Q* =

*I*. The product is

differing from an identity matrix by second order infinitesimals, discarded here. So, to first order, an infinitesimal rotation matrix is an orthogonal matrix.

Next, examine the square of the matrix,

Again discarding second order effects, note that the angle simply doubles. This hints at the most essential difference in behavior, which we can exhibit with the assistance of a second infinitesimal rotation,

Compare the products *dA*_{x}*dA*_{y} to *dA*_{y}*dA*_{x},

Since *dθ dφ* is second order, we discard it: thus, to first order, multiplication of infinitesimal rotation matrices is *commutative*. In fact,

again to first order. In other words, **the order in which infinitesimal rotations are applied is irrelevant**.

This useful fact makes, for example, derivation of rigid body rotation relatively simple. But one must always be careful to distinguish (the first order treatment of) these infinitesimal rotation matrices from both finite rotation matrices and from Lie algebra elements. When contrasting the behavior of finite rotation matrices in the BCH formula above with that of infinitesimal rotation matrices, where all the commutator terms will be second order infinitesimals one finds a bona fide vector space. Technically, this dismissal of any second order terms amounts to Group contraction.

## Realizations of rotations

{{#invoke:main|main}}

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
*S*^{3}→ SO(3) (see quaternions and spatial rotations) - in geometric algebra as a rotor

Another method is to specify an arbitrary rotation by a sequence of rotations about some fixed axes. See Euler angles.

{{#invoke:see also|seealso}}

## A note on representations

{{#invoke:main|main}} The Lie 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, , of the algebra

That is, the Casimir invariant is given by

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 2Template:Mvar+1. That is, the eigenvalues of this Casimir operator are

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

So, above, the 3×3 generators * L* displayed act on the triplet (spin 1) representation, while the the 2×2 ones (

*) act on the doublet (spin-½) representation. By taking Kronecker products of Template:Mvar 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.*

**t**For every unitary irreducible representations Template:Mvar there is an equivalent one, Template:Mvar. 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, respectively. The antihermitean matrices used above are utilized as spin operators, after they are multiplied by Template:Mvar, so they are now hermitean (like the Pauli matrices). Thus, in this language,

and hence

Explicit expressions for these Template:Mvar are,

for arbitrary Template:Mvar.

For example, the resulting spin matrices for spin 1, spin {{ safesubst:#invoke:Unsubst||$B=3/2}}, and {{ safesubst:#invoke:Unsubst||$B=5/2}} are:

(Note, however, how these are in an equivalent, but different basis than the above *i* * L*s.)

and so on.

{{#invoke:see also|seealso}}

## Generalizations

The rotation group generalizes quite naturally to *n*-dimensional Euclidean space, **R**^{n} 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 *n*(*n* − 1)/2.

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 **R**^{3}. 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 along the axis, 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)
- Euler angles
- Rodrigues' rotation formula
- Infinitesimal rotation
- Pin group
- Quaternions and spatial rotations
- Rigid body
- Spherical harmonics
- Plane of rotation
- Lie group
- Pauli matrix

## Remarks

- ↑ This is affected by first applying a rotation
*g*_{φ}through Template:Mvar about the*z*-axis to take the*x*-axis to the line*L*, the intersection between the planes*xy*and*x´y´*, the latter being the rotated*xy*-plane. Then rotate with*g*_{θ}through Template:Mvar about*L*to obtain the new*z*-axis from the old one, and finally rotate by*g*_{ψ}through an angle Template:Mvar abut the*new**z*-axis, where Template:Mvar is the angle between Template:Mvar and the new*x*-axis. In the equation,*g*_{θ}and*g*_{ψ}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**g**_{θ}=*g*_{φ}*g*_{θ}*g*_{φ}^{−1}. Here boldface means that the rotation is expressed in the*original*basis. Likewise,**g**_{ψ}=*g*_{φ}*g*_{θ}*g*_{φ}^{−1}*g*_{φ}*g*_{ψ}[*g*_{φ}*g*_{θ}*g*_{φ}^{−1}*g*_{φ}]^{-1}. Thus**g**_{ψ}**g**_{θ}**g**_{φ}=*g*_{φ}*g*_{θ}*g*_{φ}^{−1}*g*_{φ}*g*_{ψ}[*g*_{φ}*g*_{θ}*g*_{φ}^{−1}*g*_{φ}]^{-1}**g*_{φ}*g*_{θ}*g*_{φ}^{−1}**g*_{φ}=*g*_{φ}*g*_{θ}*g*_{ψ}. - ↑ For an alternative derivation of
**so**(3), see Classical group. - ↑ 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 ||
*X*|| + ||*Y*|| < log 2 and ||*Z*|| < log 2. The series may still converge even if these conditions aren't fulfilled. A solution always exists since exp is onto in the cases under consideration.

## Notes

- ↑ Jacobson (2009), p. 34, Ex. 14.
- ↑
*n*×*n*real matrices are identical to linear transformations of**R**^{n}expressed in its standard basis. - ↑ 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
- ↑ Template:Harvnb p. 95.
- ↑ Template:Harvnb
- ↑ Template:Harvnb
- ↑ See Template:Harvnb, theorem 3, section 2.2.
- ↑ Template:Harvnb Section 1.1.
- ↑ Template:Harvnb Theorem 2.27.
- ↑ Template:Harvnb
- ↑ Template:Harvnb; Template:Harvnb
- ↑ 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.
- ↑ Template:Harv

## References

- {{#invoke:citation/CS1|citation

|CitationClass=citation }}

- {{#invoke:citation/CS1|citation

|CitationClass=citation }}

- {{#invoke:citation/CS1|citation

|CitationClass=citation }}

- {{#invoke:citation/CS1|citation

|CitationClass=citation }}

- {{#invoke:citation/CS1|citation

|CitationClass=citation }}

- {{#invoke:citation/CS1|citation

|CitationClass=citation }}

- {{#invoke:citation/CS1|citation

|CitationClass=citation }}

- {{#invoke:citation/CS1|citation

|CitationClass=citation }}

- {{#invoke:citation/CS1|citation

|CitationClass=citation
}} (translation of the original 1932 edition, *Die Gruppentheoretische Methode in Der Quantenmechanik*).