The possible physical effects of general relativity on the elementary problem have usually been considered as negligible in view of the fact that energies at which the former might have a bearing are much too high. It is added that the
effects of the new particles and the energies at which current theory loses its validity occur very much below this range and therefore a correct future theory will
have solved the present difficulties in a much lower domain. In any case, field theory will have been altered so radically that arguments from the present one will lose their validity. Further, it is sometimes felt that general relativity is a purely macroscopic theory which loses its meaning in microscopic domains, where the concept of metric is not very transparent.

To these “classic” objections there exist several levels of replies. On a general level, it may be pointed out that the effect of a theory is not always first felt through its gross direct dynamical contributions (as, for example, spin). Since general relativity is needed, at least in a formal way, to provide a correct definition of the energy-momentum tensor, it underlies any theories which deal with the energies of fields and particles. The principle of general covariance on which the general theory is based is not in any way restricted *a priori* to macroscopic considerations
and it is thus necessary to explore its consequences for any theory. The fact that the metric may not be so simply measurable in microscopic domains (say “within” an elementary particle) is no more an argument against the relevance of relativity than the definition of position measurement in a hydrogen atom is an
argument against the use of coordinates in quantum mechanics. Finally, that a future correct theory will exclude the relevance of relativity is not an argument but a wish.

To these arguments of general principle, some very considerable quantitative ones can be added. The whole scheme of local field theory is plagued with divergences occurring because there is no upper limit to the energies involved in it.

For a high frequency wave packet one has roughly

Therefore, the dimensions of the wave packet must be greater than the fundamental length (
cm).

A still more significant point is the following. It is known that under very wide assumptions any theory of coupled fields leads, near the light cone, to singularities in the propagators of the “clothed” particles and to the existence of at least some infinite renormalization

This is not the case in the general theory, and it is a very basic point there. In fact, a can, as is well known, only be defined so as to be independent of any inner coordinates and therefore it cannot tell one the change of a quantity that is located somewhere in that region in question. It is connected with the non-linearity of the system and the lack of translational properties of parts of the system by themselves. One cannot simply fix the position of an arbitrary component of the total system, for this would clash with the energy density bounds mentioned above. Furthermore, matter and gravitational energies are not invariantly separable.

A second related departure from usual couplings is the form of the interaction terms. Contrary to normal field theory, there simply is no “free-particle” part of the matter Lagrangian. Here, the coupling enters in the kinetic energy, in a multiplicative fashion, and one cannot really disentangle a non-interacting particle here. This is rightly so, since the particle's mass and energy are defined precisely by the coupling. The equal time matter commutation relationships

Before one proceeds to further treat the extended theory, he must decide whether it is necessary to quantize the gravitational field.

This method will be used to determine the behavior of the matter fields as modified by gravitational interactions. It may be expected, roughly, that the contributions of the “scalar” and “transverse” parts of the gravitational field, though not really separable will limit the density of matter in a given region for the former, while for the latter will “smear out the light cone.”

The effects of gravitation on propagators of various matter fields will now be considered. Rigorously one should treat, for example, the Feynman function for an electron interacting with the electromagnetic and metric fields. However as is known, in ordinary electrodynamics in flat space the behavior of this propagator

is already singular enough to give the infinite renormalization

From the above arguments it would appear that the simplest case of a scalar field coupled to the metric is a sufficient example to consider. In the usual field theory the vacuum expectation value

where is the total action and the integration is over the meson, electron, and positron fields. The action,

Now, one can eliminate the electron field and the vacuum expectation value becomes equal to

where
is due to the pure meson field and
is due to closed loops. The Green's function

where is a well behaved function (aside from possible “harmless” logarithmic terms). Thus one finds, near the light cone, that varies essentially as . This, propagation function, , is singular enough to give one divergences.

Now consider the parallel problem when a matter field is interacting with the gravitational field.

where the D'Alembertian depends upon the metric. The mass term will, as usual, not be relevant to the singularity questions. One wants to compute

where and are to be defined with respect to a flat background frame which is used to make a classical measurement. The functional integration used to define is

where means a summation over all Riemann spaces which preserve the signature of . Now, as before, the matter variables are eliminated giving

where

and comes from integration over matter variables. One is interested only in the solution for two points which are on each other's light cones. Again, the general theory of differential equations tells one that near the light cone

where is the square of the interval between the two points and is a regular function. Here the difference between these propagators and the usual ones of field theory is obvious since the depends upon the variables. Now,

At this point the more or less rigorous mathematical treatment stops and things that are said cannot be proved mathematically.

There will be “very few” spaces where null geodesics will connect and in comparison to the number of integrations possible. It is possible to make a vague analogy to the usual theory of poles in a finite number of dimensions and in such cases one expects the singularities to be smoothed out - with any “measure” which makes sense. For large distances, on the other hand, the exponential may be expected to vary wildly and thus cancel the effects of the various spaces summed over. It is felt that one should not make the linear approximation in the action since this will reinstate the privileged character of the Minkowski metric and the whole point of non-linear gravitation is that the propagator depends upon the space one is in.

A corroborative argument from quite a different direction, which was mentioned earlier, is the commutation relation. In a flat space-time, and effectively (by suitable modification) in a non-flat but externally given geometry this commutation rule holds. determines the translation of the system as a whole and, because of superposition, of any part of it. In a space-time which interacts with matter, however, this relation no longer holds. does have as a canonical conjugate the center of mass, , of the system with respect to the flat external frame. However, it cannot be used to locate closely any component of the system. The existence of a in Minkowski space-time is essential to the pessimistic theorems mentioned before. It is obvious that if P does not have all the properties required there, the proof that any component field, if sufficiently focused on, acts as if it is uncoupled, loses support. It may be argued that the propagators, , mentioned above, also lose some of their meaning by the same argument. This is true only to the extent that physical quantities always involve space-time integrals of such functions. The fact that the are now non-singular is merely due to the fact that one can never force a field to behave as if it is too concentrated - the induced geometry would force a repulsion.

If it is granted that this action introduces an effective cutoff, at about , then such high energy approximations as Landau's could be examined again. As Landau has noted, using as a cutoff, theory predicts roughly the experimental charge regardless of the value of the bare charge and similarly for the mass. Of course, our results, being generally covariant, cannot be directly translated into flat spacetime language without apparent paradoxes.

One thing that should be done is to look into the vacuum expectation value of the total energy-momentum of the system since this should be zero in general relativity due to the absolute definition of energies; similarly, should be nowhere singular.

In the discussion which followed DESER's

A resolution was passed at this conference to the effect that there is to be another gravitational conference in Europe during the summer of 1958.

ERNST reported on a paper on Corinaldesi^{1} Here, higher order terms are obtained through a quantum treatment of the linearized theory.