# Cartan formalism (physics)

(Redirected from Cartan connection applications)

The vierbein or tetrad theory much used in theoretical physics is a special case of the application of Cartan connection in four-dimensional manifolds. It applies to metrics of any signature. (See metric tensor.) This section is an approach to tetrads, but written in general terms. In dimensions other than 4, words like triad, pentad, zweibein, fünfbein, elfbein etc. have been used. Vielbein covers all dimensions. (In German, vier means four, zwei means two, fünf means five, elf means eleven and, in general, viel means many.)

For a basis-dependent index notation, see tetrad (index notation).

## The basic ingredients

Suppose we are working on a differentiable manifold ${\displaystyle M}$  of dimension ${\displaystyle n}$ , and have fixed natural numbers ${\displaystyle p}$  and ${\displaystyle q}$  with

${\displaystyle p+q=n.}$

Furthermore, we assume that we are given an SO(p, q) principal bundle ${\displaystyle B}$  over ${\displaystyle M}$  and an SO(pq)-vector bundle ${\displaystyle V}$  associated to ${\displaystyle B}$  by means of the natural ${\displaystyle n}$ -dimensional representation of ${\displaystyle \operatorname {SO} (p,q)}$ . Equivalently, ${\displaystyle V}$  is a rank ${\displaystyle n}$  real vector bundle over ${\displaystyle M}$ , equipped with a metric ${\displaystyle \eta }$  with signature ${\displaystyle (p,q)}$  (a.k.a. non-degenerate quadratic form).[1]

The basic ingredient of the Cartan formalism is an invertible linear map ${\displaystyle e\colon {V}\to \operatorname {T} M}$ , between vector bundles over ${\displaystyle M}$  where TM is the tangent bundle of ${\displaystyle M}$ . The invertibility condition on ${\displaystyle e}$  is sometimes dropped. In particular if ${\displaystyle B}$  is the trivial bundle, as we can always assume locally, V has a basis of orthogonal sections ${\displaystyle f_{a}=f_{1}\ldots f_{n}}$ . With respect to this basis ${\displaystyle \eta _{ab}=\eta (f_{a},f_{b})=\operatorname {diag} (1,\ldots 1,-1,\ldots ,-1)}$  is a constant matrix. For a choice of local coordinates ${\displaystyle x^{\mu }=x^{-1},\ldots ,x^{-n}}$  on ${\displaystyle M}$  (the negative indices are only to distinguish them from the indices labeling the ${\displaystyle f_{a}}$ ) and a corresponding local frame ${\displaystyle \textstyle \partial _{\mu }={\frac {\partial }{\partial x^{\mu }}}}$  of the tangent bundle, the map ${\displaystyle e}$  is determined by the images of the basis sections

${\displaystyle e_{a}:=e(f_{a}):=e_{a}^{\mu }\partial _{\mu }.}$

They determine a (non coordinate) basis of the tangent bundle (provided ${\displaystyle e}$  is invertible and only locally if ${\displaystyle B}$  is only locally trivialised). The matrix ${\displaystyle e_{a}^{\mu },\mu =-1,\dots ,-n,a=1,\dots ,n}$  is called the tetrad, vierbein, vielbein, etc. Its interpretation as a local frame crucially depends on the implicit choice of local bases.

Note that an isomorphism ${\displaystyle V\cong \operatorname {T} M}$  gives a reduction ${\displaystyle B\to \operatorname {Fr} (M)}$  of the frame bundle, the principal bundle of the tangent bundle. In general, such a reduction is impossible for topological reasons. Thus, in general for continuous maps ${\displaystyle e}$ , one cannot avoid that ${\displaystyle e}$  becomes degenerate at some points of ${\displaystyle M}$ .

## Example: general relativity

We can describe geometries in general relativity in terms of a tetrad field instead of the usual metric tensor field. The metric tensor ${\displaystyle g_{\alpha \beta }}$  gives the inner product in the tangent space directly:

${\displaystyle \langle \mathbf {x} ,\mathbf {y} \rangle =g_{\alpha \beta }\,x^{\alpha }\,y^{\beta }.\,}$

The tetrad ${\displaystyle e_{\alpha }^{i}}$  may be seen as a (linear) map from the tangent space to Minkowski space that preserves the inner product. This lets us find the inner product in the tangent space by mapping our two vectors into Minkowski space and taking the usual inner product there:

${\displaystyle \langle \mathbf {x} ,\mathbf {y} \rangle =\eta _{ij}(e_{\alpha }^{i}\,x^{\alpha })(e_{\beta }^{j}\,y^{\beta }).\,}$

Here ${\displaystyle \alpha }$  and ${\displaystyle \beta }$  range over tangent-space coordinates, while ${\displaystyle i}$  and ${\displaystyle j}$  range over Minkowski coordinates. The tetrad field ${\displaystyle e_{\alpha }^{i}(\mathbf {x} )}$  defines a metric tensor field via the pullback ${\displaystyle g_{\alpha \beta }(\mathbf {x} )=\eta _{ij}\,e_{\alpha }^{i}(\mathbf {x} )\,e_{\beta }^{j}(\mathbf {x} )}$ .

## Constructions

A (pseudo-)Riemannian metric is defined over ${\displaystyle M}$  as the pullback of ${\displaystyle \eta }$  by ${\displaystyle e}$ . To put it in other words, if we have two sections of ${\displaystyle \mathrm {T} M}$ , ${\displaystyle \mathbf {X} }$  and ${\displaystyle \mathbf {Y} }$ ,

${\displaystyle g(\mathbf {X} ,\mathbf {Y} )=\eta (e(\mathbf {X} ),e(\mathbf {Y} )).}$

A connection over ${\displaystyle V}$  is defined as the unique connection ${\displaystyle \mathbf {A} }$  satisfying these two conditions:

• ${\displaystyle d\eta (a,b)=\eta (d_{\mathbf {A} }a,b)+\eta (a,d_{\mathbf {A} }b)}$  for all differentiable sections ${\displaystyle a}$  and ${\displaystyle b}$  of ${\displaystyle V}$  (i.e. ${\displaystyle d_{\mathbf {A} }\eta =0}$ ) where ${\displaystyle d_{\mathbf {A} }}$  is the covariant exterior derivative. This implies that ${\displaystyle \mathbf {A} }$  can be extended to a connection over the ${\displaystyle \operatorname {SO} (p,q)}$  principal bundle.
• ${\displaystyle d_{\mathbf {A} }e=0}$ . The quantity on the left hand side is called the torsion. This basically states that ${\displaystyle \nabla }$  defined below is torsion-free. This condition is dropped in the Einstein–Cartan theory, but then we cannot define ${\displaystyle \mathbf {A} }$  uniquely anymore.

This is called the spin connection.

Now that we have specified ${\displaystyle \mathbf {A} }$ , we can use it to define a connection ${\displaystyle \nabla }$  over ${\displaystyle \mathrm {T} M}$  via the isomorphism ${\displaystyle e}$ :

${\displaystyle e(\nabla \mathbf {X} )=d_{\mathbf {A} }e(\mathbf {X} )}$  for all differentiable sections ${\displaystyle \mathbf {X} }$  of ${\displaystyle \mathrm {T} M}$ .

Since what we now have here is a ${\displaystyle \operatorname {SO} (p,q)}$  gauge theory, the curvature ${\displaystyle \mathbf {F} }$  defined as ${\displaystyle \mathbf {F} \ {\stackrel {\mathrm {def} }{=}}\ d\mathbf {A} +\mathbf {A} \wedge \mathbf {A} }$  is pointwise gauge covariant. This is simply the Riemann curvature tensor in a different form.

An alternate notation writes the connection form ${\displaystyle \mathbf {A} }$  as ${\displaystyle \omega }$ , the curvature form ${\displaystyle \mathbf {F} }$  as ${\displaystyle \Omega }$ , the canonical vector-valued 1-form ${\displaystyle e}$  as ${\displaystyle \theta }$ , and the exterior covariant derivative ${\displaystyle d_{\mathbf {A} }}$  as ${\displaystyle D}$ .

## The Palatini action

In the tetrad formulation of general relativity, the action, as a functional of the vierbein ${\displaystyle e}$  and a connection form ${\displaystyle \omega }$ , with an associated field strength ${\displaystyle \Omega =D\omega =d\omega +\omega \wedge \omega }$ , over a four-dimensional differentiable manifold ${\displaystyle M}$  is given by

{\displaystyle {\begin{aligned}S\,\,&{\stackrel {\mathrm {def} }{=}}\ M_{pl}^{2}\int _{M}\varepsilon _{abcd}(e^{a}\wedge e^{b}\wedge \Omega ^{cd})=M_{pl}^{2}\int _{M}d^{4}x\,\varepsilon ^{\mu \nu \rho \sigma }\varepsilon _{abcd}e_{\mu }^{a}e_{\nu }^{b}R_{\rho \sigma }^{cd}[\omega ]\\[5pt]&=M_{pl}^{2}\int |e|d^{4}x\,{\frac {1}{2}}e_{a}^{\mu }e_{b}^{\nu }R_{\mu \nu }^{ab}\\[5pt]&={\frac {c^{4}}{16\pi G}}\int d^{4}x\,{\sqrt {-g}}R[g]\end{aligned}}}

where ${\displaystyle \Omega _{\mu \nu }^{ab}=R_{\mu \nu }^{ab}}$  is the gauge curvature 2-form, ${\displaystyle \varepsilon _{abcd}}$  is the antisymmetric Levi-Civita symbol, and that ${\displaystyle |e|=\varepsilon ^{\mu \nu \rho \sigma }\varepsilon _{abcd}e_{\mu }^{a}e_{\nu }^{b}e_{\rho }^{c}e_{\sigma }^{d}}$  is the determinant of ${\displaystyle e_{\mu }^{a}}$ . Here we see that the differential form language leads to an equivalent action to that of the normal Einstein–Hilbert action, using the relations ${\displaystyle |e|={\sqrt {-g}}}$  and ${\displaystyle R_{\mu \nu }^{\lambda \sigma }=e_{a}^{\lambda }e_{b}^{\sigma }R_{\mu \nu }^{ab}}$ . Note that in terms of the Planck mass, we set ${\displaystyle \hbar =c=1}$ , whereas the last term keeps all the SI unit factors.

Note that in the presence of spinor fields, the Palatini action implies that ${\displaystyle d\omega }$  is nonzero. So there's a non-zero torsion, i.e. that ${\displaystyle {\hat {\omega }}_{\mu }^{ab}=\omega _{\mu }^{ab}+K_{\mu }^{ab}}$ . See Einstein–Cartan theory.

## Notes

1. ^ A variant of the construction uses reduction to a Spin(pq) principal spin bundle. In that case, the principal bundle contains more information than the bundle V together with the metric η, which is needed to construct spinorial fields.