The issue of gauge invariance, the understanding of which is not obvious or easy, must now be addressed. The claim is that the work described here is in fact gauge (or BMS) invariant.
First of all we have, , or its real part, . On , for each choice of spacetime interior and solution of the Einstein–Maxwell equations, we have its UCF, either in its complex version, , or its real version, Equation (291). The geometric picture of the UCF is a one-parameter family of slicings (complex or real) of or . This is a geometric construct that has a different appearance or description in different Bondi coordinate systems. It is this difference that we must investigate. We concentrate on the complex version.
Under the action of the supertranslation, Equation (67), we have:
The action of the homogeneous Lorentz transformations, Equation (68),
Before discussing the relevant effects of the Lorentz transformations on our considerations we first digress and describe an important technical issue concerning representation of the homogeneous Lorentz group.
The representation theory of the Lorentz group, developed and described by Gelfand, Graev and Vilenkin  used homogeneous functions of two complex variables (homogeneous of degrees, and ) as the representation space. Here we summarize these ideas via an equivalent method [21, 15] using spin-weighted functions on the sphere as the representation spaces. In the notation of Gelfand, Graev and Vilenkin, representations are labeled by the two numbers or by , with . The ‘’ is the same ‘’ as in the spin weighted functions and ‘’ is the conformal weight  (sometimes called ‘boost weight’). The different representations are written as . The special case of irreducible unitary representations, which occur when are not integers, play no role for us and will not be discussed. We consider only the case when are integers so that the take integer or half integer values. If and are both positive integers or both negative integers, we have, respectively, the positive or negative integer representations. The representation space, for each , are the functions on the sphere, , that can be expanded in spin-weighted spherical harmonics, , so that
Under the action of the Lorentz group, Equation (335), they transform asIt is this fact which we heavily utilize. More specifically we have two related situations: (1) when the are both positive integers, (or ), there will be finite dimensional invariant subspaces, , which are spanned by the basis vectors , with given in the range, . All the finite dimensional representations can be obtained in this manner. And (2) when the are both negative integers (i.e., we have a negative integer representation) there will be an infinite dimensional invariant subspace, , described elsewhere . One, however, can obtain a finite dimensional representation for each negative integer case by the following construction: One forms the factor space, . This space is isomorphic to one of the finite dimensional spaces associated with the positive integers. The explicit form of the isomorphism, which is not needed here, is given in Held et al. [21, 16].
Of major interest for us is not so-much the invariant subspaces but instead their interactions with their compliments (the full vector space modulo the invariant subspace). Under the action of the Lorentz transformations applied to a general vector in the representation space, the components of the invariant subspaces remain in the invariant subspace but in addition components of the complement move into the invariant subspace. On the other hand, the components of the invariant subspaces do not move into the complement subspace: the transformed components of the compliment involve only the original compliment components. The transformation thus has a non-trival Jordan form.
Rather than give the full description of these invariant subspaces we confine ourselves to the few cases of relevance to us.
I. Though our interest is primarily in the negative integer representations, we first address the positive integer case of the and , , representation. The harmonics, form the invariant subspace. The cut function, , for each fix values of , lies in this space.
We write the GCF as
After the Lorentz transformation, the geometric slicings have not changed but their description in terms of has changed to that of . This leads to
Using the transformation properties of the invariant subspace and its compliment we see that the coordinate transformation must have the form;
Treating the and as functions of , we haveare the coefficients of the harmonics in respectively the and the expansions. A Lorentz transformation induces a specific coordinate transformation and associated vector transformation on these coefficients.
II. A second important example concerns the mass aspect, (where we have introduced the for simplicity of treatment of numerical factors)isomorphic to the finite dimensional positive integer space, and hence the harmonic coefficients of ) lie in this finite dimensional representation space. From this isomorphism we know that functions of the form, , have four coefficients proportional to the Bondi four-momentum
This is the justification for calling the harmonics of the mass aspect a Lorentzian four-vector. Technically, the Bondi four-momentum is a co-vector but we have allowed ourselves a slight notational irregularity.
III. The Weyl tensor component, , has and , . The associated finite dimensional factor space is isomorphic to the finite part of the representation. We have that
The question of what finite tensor transformation this corresponds to is slightly more complicated than that of the previous examples of Lorentzian vectors. In fact, it corresponds to the Lorentz transformations applied to (complex) self-dual antisymmetric two-index tensors . We clarify this with an example from Maxwell theory: from a given E and B, the Maxwell tensor, , and then its self-dual version can be constructed:
A Lorentz transformation applied to the tensor, , is equivalent  to the same transformation applied to
These observations allow us to assign Lorentzian invariant physical meaning to our identifications of the Bondi momentum, and the complex mass dipole moment and angular momentum vector, .
IV. Our last example is a general discussion of how to construct Lorentzian invariants from the representation spaces. Though we will confine our remarks to just the cases of , it is easy to extend them to non-vanishing by having the two functions have respectively spin-weight and .
Consider pairs of conformally weighted functions (), , with weights respectively, . They are considered to be in dual spaces. Our claim is that the integrals of the form
We first point out that under the fractional linear transformation, , Equation (337), the area element on the sphere
This leads immediately to
There are several immediate simple applications of Equation (352). By choosing an arbitrary function, say , we immediately have a Lorentzian scalar,
If this is made more specific by chosing , we have the remarkable result (proved in Appendix D) that this scalar yields the -space metric via
A simple variant of this arises by taking the derivative of (357) with respect to and multiplying by an arbitrary vector, leading to
Many other versions can easily be found.
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