Abelian-Higgs strings in Rastall gravity

Abelian-Higgs strings in Rastall gravity

Eugênio R. Bezerra de Mello emello@fisica.ufpb.br    Júlio C. Fabris fabris@pq.cnpq.br    Betti Hartmann bettihartmann@googlemail.com Departamento de Física, Universidade Federal da Paraíba, 58.059-970, Caixa Postal 5.008, João Pessoa, PB, Brazil
Universidade Federal do Espírito Santo, Departamento de Física, CEP 29075-910, Vitória (ES), Brazil
School of Engineering and Science, Jacobs University Bremen, 28759 Bremen, Germany
July 14, 2019
Abstract

In this paper we analyze Abelian-Higgs strings in a phenomenological model that takes quantum effects in curved space-time into account. This model, first introduced by Rastall, cannot be derived from an action principle. We formulate phenomenological equations of motion under the guiding principle of minimal possible deformation of the standard equations. We construct string solutions that asymptote to a flat space-time with a deficit angle by solving the set of coupled non-linear ordinary differential equations numerically. Decreasing the Rastall parameter from its Einstein gravity value we find that the deficit angle of the space-time increases and becomes equal to at some critical value of this parameter that depends on the remaining couplings in the model. For smaller values the resulting solutions are supermassive string solutions possessing a singularity at a finite distance from the string core. Assuming the Higgs boson mass to be on the order of the gauge boson mass we find that also in Rastall gravity this happens only when the symmetry breaking scale is on the order of the Planck mass. We also observe that for specific values of the parameters in the model the energy per unit length becomes proportional to the winding number, i.e. the degree of the map . Unlike in the BPS limit in Einstein gravity, this is, however, not connect to an underlying mathematical structure, but rather constitutes a would-be-BPS bound.

pacs:
98.80.Cq, 11.27.+d

I Introduction

One of the well-known ingredients of Einstein’s theory of General Relativity is the covariant conservation of the energy-momentum tensor which leads, via Noether’s Theorem, to the conservation of globally defined quantities. These quantities appear as integrals of the components of the energy-momentum tensor over suitable space-like surfaces that typically have one of the Killing vectors of the space-time as their normal. As such, the total rest energy/mass of a system is conserved in General Relativity. Now the question is whether this is a suitable assumption as there is (up to date) no clear experimental evidence for this. Hence, models have been developed that relax the condition of covariant energy-momentum conservation. In this paper we are interested in a modification of General Relativity suggested by Rastall Rastall:1973nw (). In this model, the gravitational fields are sourced by the energy and momentum, as in General Relativity, but also by the metric of the external space. Since in empty space, i.e. for a vanishing energy-momentum tensor Rastall gravity agrees with General Relativity, this can be seen as a direct implementation of Mach’s principle stating that the inertia of a mass distribution should be dependent on the mass and energy of the external space-time Majernik:2006jg (). This model has been studied extensively in the context of cosmology Batista:2012hv (); Fabris:2012hw (); Batista:2011nu ().

At first sight Rastall’s theory has major drawbacks: its phenomenological formulation and in addition the absence of a variational principle. However, it contains a rich structure that may be easily connected with many fundamental aspects of a gravity theory. First of all, the usual energy-momentum conservation law of Special Relativity may be generalized to curved space-time in many different ways, including geometric terms. General Relativity is one possible extension and constitutes a minimal implementation of such a generalization by replacing the standard derivative with a covariant derivative. This by itself is not completely free of unclear aspects. On the other hand, if quantum effects are taken into account in curved space-time the classical expression for the energy-momentum tensor must be modified introducing quantities related to the curvature of the space-time bd (). Moreover, the propagation of quantum fields in space-times with horizons may lead to a violation of the classical conservation law (due to the chirality of the quantum modes) leading to a so-called gravitational anomaly anomalias (). In this sense, Rastall’s theory is a phenomenological procedure to consider effects of quantum fields in curved space-time and to investigate in a completely covariant way such effects. Even if there is in principle no action leading to the Rastall equation it is possible to find such an action if an external field is introduced in the Einstein-Hilbert action through a Lagrange multiplier. This is somehow a reminiscence of the quantum effects described by the Rastall equation. Other geometrical frameworks, like Weyl geometry, may lead to equations similar to the ones in Rastall gravity smalley (); romero ().

In this paper we are interested in static, cylindrically symmetric solutions to the Rastall gravity model coupled to the U(1) Abelian-Higgs model. These solutions constitute field theoretical realizations of a specific type of topological defect called Abelian-Higgs string no () which could e.g. describe infinite straight cosmic strings whose properties have been analyzed in DG (); Laguna (). Topological defects are believed to have formed in the numerous phase transitions in the early universe due to the Kibble mechanism topological_defects (). While magnetic monopoles and domain walls, which result from the spontaneous symmetry breaking of a spherical and parity symmetry, respectively, are catastrophic for the universe since they would overclose it, cosmic strings are an acceptable remnant from the early universe. These objects form whenever an axial symmetry gets spontaneously broken and, due to topological arguments, are either infinitely long or exist in the form of cosmic string loops. Numerical simulations of the evolution of cosmic string networks have shown that these networks reach a scaling solution, i.e. their contribution to the total energy density of the universe becomes constant at some stage. The main mechanism that allows cosmic string networks to reach this scaling solution is the formation of cosmic string loops due to self-intersection and the consequent decay of these loops under the emission of gravitational radiation.

For some time, cosmic strings were believed to be responsible for the structure formation in the universe. New Cosmic Microwave Background (CMB) data clearly shows that the theoretical power spectrum associated to cosmic strings is in stark contrast to the observed power spectrum. However, other effects might be caused by moving cosmic strings that can potentially be observed in the CMB data (see e.g. Planck () for a recent discussion). Moreover, there has been a recent revival of cosmic strings since it is now believed that cosmic strings might be linked to the fundamental strings of String Theory polchinski (). While perturbative fundamental strings were excluded to be observable on cosmic scales for many reasons witten (), there are now new theories containing extra dimensions, so-called brane world model, that allow to lower the fundamental Planck scale down to the TeV scale. Moreover, cosmic strings are interesting due to the recent BICEP2 data bicep () that showed evidence for a B-mode polarization at small in the Cosmic Microwave background (CMB). While topological defects cannot be accounted for the B-mode polarization alone Lizarraga:2014eaa () it has been suggested that this polarization results from gravitational waves, i.e. tensor modes, originating from an inflationary epoch in the early universe. If that turns out to be correct the question remains what the origin of the field driving inflation is and how it can be embedded into suitable Unified Theories, which are certainly necessary to describe the physics at the energy scales relevant for the inflationary epoch. Now, it is interesting that cosmic strings generically form at the end of inflation in inflationary models resulting from String Theory braneinflation () and Supersymmetric Grand Unified Theories susyguts (). Hence, it is conceivable that cosmic strings show up in the CMB and, indeed, CMB data (power and polarization spectra) are well compatible with a substantial amount of the total energy density of the universe coming from cosmic strings cmb (); cmb2 ().

While field theoretical cosmic strings would always form loops when self-intersecting (and hence providing a “short-cut” for the magnetic flux), this can well be different for cosmic superstrings. The question then is how these networks of cosmic superstrings loose energy to reach a scaling solution and hence be not dangerous for the universe today. One of the suggestions is that they can form bound states. Since it is difficult to study cosmic superstrings with respect to the formation of bound states, the interaction of cosmic strings has been investigated in the context of field theoretical models describing bound systems of D- and F-strings, so-called p-q-strings saffin (); hu ().

In order to understand the lensing properties of cosmic strings (and hence their impact on the CMB spectrum) as well as the evolution of cosmic string networks in different gravity models it is important to study their properties in detail. This is the aim of this paper which considers cosmic string in the Rastall gravity model.

Our paper is organized as follows: In Section II, we briefly introduce the gravity model proposed by Rastall. In Section III we present the U(1) Abelian-Higgs model that we study coupled to Rastall gravity. We present the set of differential equations associated with this system and give the asymptotic behavior for the matter and for the metric functions. In Section IV we present our numerical results. In section V we give our conclusions. The Appendix contains an outline on the procedure we used to derive the equations of motion for the matter fields.

Ii The model

Rastall’s generalization of General Relativity Rastall:1973nw () uses the idea of covariant non-conservation of the energy-momentum tensor and has been cast into the following form (where )

(1)

or

(2)

where denotes the covariant derivative, the energy-momentum tensor with trace and the Ricci scalar. and are some coupling constants such that in the limit we recover standard Einstein gravity. Note that the equations above imply a violation of the principle of General Covariance.

The equations for Rastall gravity and the violation of the conservation of energy-momentum tensor then read

(3)

and

(4)

Of course the constants , and can be easily related and corresponds to the Einstein gravity limit.

The equations (3) and (4) can be written in the form

(5)

and

(6)

where are the Christoffel symbols.

Iii Abelian-Higgs strings

In this section we would like to study Abelian-Higgs strings in Rastall gravity. The matter Lagrangian density, , is given by

(7)

with the covariant derivative = - of the complex scalar field . The field strength tensor is , of the U(1) gauge potential with coupling constant . denotes the gravitational covariant derivative. Finally, is the self-coupling of the scalar field, while denotes the vacuum expectation value. We define the energy momentum tensor to be given in the standard way by the variation of the matter Lagrangian with respect to the metric

(8)

Note, however, that this is not linked to an action principle in which the variation of the total action (matter plus metric) with respect to the metric gives the gravity equations. The model we are studying here is a phenomenological model in which we insert “by hand” the non-conservation of the energy-momentum tensor.

The symmetry breaking pattern is such that and the scalar field as well as the gauge field acquire mass: the Higgs field has mass , while the gauge boson mass is .

By using the standard cylindrical coordinates , the most general static cylindrically symmetric line element invariant under boosts along the -direction is:

(9)

where and are functions of only.

The non-vanishing components of the Ricci tensor then read clv ():

(10)

where the prime now and in the following denotes the derivative with respect to .

For the matter and gauge fields, we have no ()

(11)

where is an integer indexing the vorticity of the Higgs field around the axis, i.e. corresponds to the degree of the map . In the following we will study only the case .

Now let us define the following dimensionless quantities

(12)

such that measures the radial distance in units of . Then, the Lagrangian density, , depends only on the following dimensionless coupling constants

(13)

where is the Planck mass.

The non-vanishing components of the energy-momentum tensor read clv ()

(14)
(15)
(16)

and the trace is given by

(17)

Now, since the trace of the energy-momentum tensor is independent of the and the coordinate we have

(18)

Note that this is not a consequence of the gravity model used, as it would be in General Relativity, but rather a consequence of the particular choice of the matter content. Then, (18) allows us to define globally conserved charges, namely the energy per unit length, , as well as the tension along the string axis, , in the usual way (with denoting the determinant of the induced metric on spatial sections perpendicular to )

(19)

where obviously from the fact that we find that . Note that we “measure” in units of . A quantity often cited when discussing the observational effects of cosmic strings is , where is the dimensionful energy per unit length of the string. This quantity enters in both the expression for the deficit angle as well as the temperature anisotropies in the CMB. In our dimensionless units the quantity is equal to .

iii.1 Equations of motion

We use the - and -components of the Rastall equation (5):

(20)

and

(21)

The component reads

(22)

which can be combined with (20) and (21) to obtain a constraint that is first order in derivatives

(23)

Finally, the modified conservation law (6) reads

(24)

For we can derive the Euler-Lagrange equations by the variation of the action with respect to the matter fields. This is not possible here, hence we “read-off” the equations from the conservation law (24). This is motivated by the fact that in standard Einstein gravity the conservation law holds on shell, i.e. for solutions of the Euler-Lagrange equations. Moreover, we require that the equations become equal to the standard equations in the limit and constitute a minimal extension of the given model (see also the Appendix).

It hence makes sense to consider the following equations of motion for the matter fields:

(25)

and

(26)

Note that these, indeed, reduce to the standard Euler-Lagrange equations in the limit .

Hence we have to solve a system of four coupled, non-linear ordinary differential equations numerically subject to appropriate boundary conditions. These read

(27)

to ensure regularity on the -axis. Furthermore, we want the matter fields to reach their vacuum expectation values asymptotically. So, we require

(28)

iii.2 Behaviour close to the string axis

The behaviour at is determined by the requirement of imposing globally regular solutions. From the boundary conditions it follows for the metric functions

(29)

where is a constant.

Inserting this into (25) we find the following behaviour of at small

(30)

For this reduces to , but here the behaviour is much more complicated and depends strongly on . In particular we note that we have to require in order to have regular solutions. For the gauge field we find

(31)

Consequently, the behaviour of the gauge field at the origin does not depend on .

iii.3 Asymptotic behaviour

In the absence of matter sources, Rastall gravity reduces to standard Einstein gravity. Since the energy-momentum tensor associated with the matter fields in our model falls off exponentially fast and since we want the Abelian-Higgs string to be well-localized, we can assume that far away from the string core the space-time corresponds to a cylindrical vacuum space-time. Now, it is well known that cylindrical solutions of the vacuum Einstein equations are of the Kasner type. Hence, we would expect our solutions to asymptote to these such that the fall-off of the metric functions is

(32)

where the coefficients and have to fulfill the Kasner conditions

(33)

with and being constants. The two possible solutions to (33) are

(34)

The first set of parameters corresponds to string-like solutions, in which case determines the deficit angle of the space-time. The second set of possible values are the so-called Melvin solutions, which are not of physical interest in cosmological settings, however are mathematical solutions to the equations of motion. The string-like solution then possesses a deficit angle which can be expressed as follows:

(35)

The matter field functions have the following behaviour at

(36)

and

(37)

where and are constants and and correspond to the effective Higgs and gauge boson mass, respectively. For the Higgs field reaches its vacuum value quicker than the gauge field if and slower if . The value corresponds to the BPS limit. In this limit the masses of the gauge and Higgs bosons are equal. Now for this changes. The effective Higgs and gauge boson mass are equal for , which is equal unity for and decreases monotonically with decreasing .

Iv Numerical results

To the best of our knowledge there are no explicit solutions to the set of coupled differential equations presented above. We have hence solved the equations numerically using the ODE solver COLSYS colsys (). Relative errors of the solutions are typically on the order of to (and sometimes even better).

The limit corresponds to standard Einstein gravity. From (25) it is apparent that is excluded. Furthermore, we see from (30) that in order for the solutions at , where is small, to behave like the solutions in the limit we must choose the positive sign. This means that for the parameter . However, since we need to require at , otherwise the space-time would not be regular, this leads to infinities on the right hand side of the gravity equations (20) and (21). So, we conclude that we have to choose .

For it is well known that the coupled system of equations admits gravitating Abelian-Higgs string solutions. In this paper we are interested to investigate the influence of the Rastall parameter, , on the behavior of the matter fields and on the metric. Since Rastall gravity reduces to Einstein gravity in the absence of sources our asymptotic space-time (in which the matter fields reach their vacuum values) should be a solution to Einstein gravity. We can hence use the standard definition of a deficit angle given in (35).

Let us first recall what is know about the Einstein gravity case . In this case, it has been observed that the value of depends on both and and increases with increasing . At some maximal value of the deficit angle becomes equal to . For no globally regular string solutions exist, but only solutions with singularities (so-called “supermassive” or “inverted” string solutions). These supermassive solutions possess a singularity at some finite value of the radial coordinate at which , while stays finite clv (); Brihaye:2000qr ().

In Fig.1 we show the behavior of a typical Abelian-Higgs string solution for and and different values of . For and these solutions fulfill a Bogomolnyi-Prasad-Sommerfield (BPS) bound. In this limit the components of the energy-momentum tensor in the direction perpendicular to the string axis vanish implying via (20) that . This means that there is no gravitational force acting perpendicular to the string axis. In this limit, the remaining equations can be recast into the form

(38)

A solution of this type is shown in Fig.1. Decreasing the Rastall parameter we observe that both the gauge field function as well as the Higgs field function are stronger localized around the string axis implying that the width of the string decreases. At the same time, the metric function starts to deviate from its constant value of unity stronger and stronger when decreasing . Furthermore, the metric function possesses a decreasing slope at large implying an increase in the deficit angle with decreasing . This seems natural since the energy-momentum content is localized inside a smaller region of space-time.

(a) gauge field function
(b) Higgs field function
(c) metric function
(d) metric function
Figure 1: We show the profiles of the matter functions and (top) and the metric functions and (bottom) for Abelian-Higgs strings in Rastall gravity with and . The curves correspond to the Einstein gravity limit, while the case gives the profiles of the solution which has .

Let us now discuss the value of the deficit angle, , in more detail since this is an important quantity when predicting observational consequences of strings. The deficit angle leads to gravitational lensing as well as to red-and blue-shift of photons towards which and away from which, respectively, the string is moving (the Kaiser-Stebbins effect). Strings (if they existed) would hence have an important impact on the temperature anisotropies of the CMB. It is often stated that the deficit angle . This is strictly speaking only true in the BPS limit . In this case, it is easy to see from (38) and the definition of that this relation indeed holds. Since furthermore in this limit, the energy per unit length in the BPS limit is we find that the deficit angle in this specific case is .

We have studied the case and , and , respectively. Our results are shown in Fig.2, where we give the deficit angle as function of . The function stays finite all along and varies only little. This is why we do not present any detailed results about it here.

Figure 2: We show the value of the deficit angle in dependence on for and different values of .

For the deficit angle has the known value (see e.g.Brihaye:2000qr ()). E.g. in the BPS limit, , we have . Decreasing we find that the deficit increases until it reaches at some value of . For the solutions have a singularity at a finite value of the radial coordinate with .

The critical value for depends on the value of . Considering , we observe that for the critical value is , while for we have . For we find that the deficit angle stays smaller than for all values of . The results for are shown in Fig.3. For we find that non-singular string solutions exist for all values of . For increasing the value of increases, but reaches only exponentially slow. Hence, we find that for all reasonable values of the Higgs to gauge boson mass ratio as well as the ratio between the symmetry breaking scale and the Planck mass regular Abelian-Higgs strings in Rastall gravity can be constructed.

Figure 3: We show the value of in dependence on for three different values of . String solutions with deficit angle smaller than and hence without singularity exist only for values of above the curve.

As stated above, for and/or there is no linear relation between the deficit angle and the energy per unit length . We have hence also studied the energy per unit length in dependence on the parameters of the model. Our results are shown in Fig.4.

Figure 4: We show the value of the energy per unit length in dependence on for three different values of and two different values of , respectively.

As is clearly seen from this figure, we have for . For the other cases, the energy per unit length still depends (nearly) linearly on and behaves as

(39)

where is a function that depends on and and fulfills the condition . Now, we find that this function is monotonically increasing with and becomes nearly constant for very large values of . For it is negative, while for it is positive in the Einstein gravity limit . This function also increases with decreasing , i.e. moving away more and more from the Einstein gravity limit. The increase is stronger for larger values of . Now, we can make an interesting observation. If we choose , we can find values of for which , i.e. corresponding to the energy per unit length that the solution has in the BPS limit in standard Einstein gravity. In the following we will refer to this as a would-be-BPS limit. For this is true for all values of . For a fixed value of and we can then decrease such that at some specific value of , the energy per unit length becomes again equal to unity (in units of ). We find that the lower the lower we have to choose to achieve this condition. E.g. for we find that for , while for . We also find a (albeit smaller) dependence on . E.g. for we find for . Hence, decreases with increasing .

V Conclusions

In this paper we have studied Abelian-Higgs strings in the context of Rastall gravity. Rastall theory touches one of the cornerstones of General Relativity, namely the conservation of the energy-momentum tensor. The violation of the conservation law is parametrized in terms of a parameter with constituting the General Relativity limit. In spite of its phenomenological character Rastall gravity may be related to an effective (and hence classical) implementation of a gravitational anomaly that might appear due to quantum effects. Our main purpose here was to investigate the impact of these effects on a field theoretical realization of line-like topological defects, so-called cosmic strings. Our main results can be summarized as follows:

  • we find that singularity-free space-times are possible only when ,

  • depending on the other parameters in the model (the two ratios between the fundamental mass scales) the solid deficit angle becomes equal to at a value of ,

  • a BPS limit in which the energy per unit length saturates a bound (and hence becomes equal to ) does not seem to exist here unlike for the Einstein gravity limit, where it exists for equal gauge and Higgs boson mass,

  • a would-be-BPS bound exists at which the energy per unit length becomes equal to , i.e. fulfills the above mentioned bound. However, this is not related to an underlying mathematical structure.

Our results are interesting because of the recently presented BICEP2 data. If the measurements of the B-mode polarization are confirmed (preferably additionally through other measurements like e.g. the PLANCK collaboration) we do have a window to the very early universe and the phase of inflation. Now inflation seems to be driven by scalar fields and the question remains where these originate from. Most unifying models that are able to model inflation predict the production of cosmic strings at the end of inflation. Hence, it might turn out that if inflation took place, cosmic strings become a prediction rather than a speculation. Since it is certain that the energy conditions at the epoch of inflation are extreme, we would expect that quantum effects play a rôle (even if one treats the gravity side classically this can certainly not be said for the matter side). Rastall gravity is one possibility to model these quantum effects effectively. Our results presented above suggest that taking such corrections into account could have stronger effects on the CMB due to an increased deficit angle.

While in this paper we have studied string-like objects without additional structure one could also think of investigating strings with additional degrees of freedom inside their core. These could be in the form of fermionic or bosonic currents and the corresponding objects have been coined superconducting strings witten2 (). Since the stability of these objects is of huge importance in the context of the formation of loops of cosmic string, so-called vortons (see e.g. peter_uzan () for more details) a macroscopic stability criterion has been developed carter (); carter2 () and used in a detailed analysis for superconducting string solutions of the U(1) U(1) model in flat space-time patrick3 () as well as in curved space-time hartmann_michel (). It would be very interesting to study possible quantum effects on the stability of these objects and the Rastall gravity model would implement these quantum effects naturally. Acknowledgment B.H. would like to acknowledge the CNPq for financial support. B.H. would also like to acknowledge the Deutsche Forschungsgemeinschaft (DFG) for support within the framework of the DFG Research Group 1620 Models of Gravity. E.R.B.M. and J.C.F. would also like to acknowledge CNPq and FAPES for partial financial support.

References

  • (1) P. Rastall, Phys. Rev. D 6 3357 (1972).
  • (2) V. Majernik and L. Richterek, Rastall’s gravity equations and Mach’s principle, gr-qc/0610070.
  • (3) C. E. M. Batista, J. C. Fabris, O. F. Piattella and A. M. Velasquez-Toribio, Eur. Phys. J. C 73 2425 (2013).
  • (4) J. C. Fabris, O. F. Piattella, D. C. Rodrigues, C. E. M. Batista and M. H. Daouda, Int. J. Mod. Phys. Conf. Ser. 18 67 (2012).
  • (5) C. E. M. Batista, M. H. Daouda, J. C. Fabris, O. F. Piattella and D. C. Rodrigues, Phys. Rev. D 85 084008 (2012).
  • (6) N. D. Birrell and P. C. W. Davies, Quantum fields in curved space, Cambridge University Press, Cambridge (1982).
  • (7) R. Bertlmann, Anomalies in Quantum Field Theory, Oxford University Press, Oxford (2000).
  • (8) L. L. Smalley, Nuovo Cim. B 80 42 (1984).
  • (9) T. S. Almeida, M. L. Pucheu, C. Romero and J. B. Formiga, Phys. Rev. D 89 064047 (2014).
  • (10) H. B. Nielsen and P. Olesen, Nucl. Phys. B 61, 45 (1973).
  • (11) D. Garfinkle, Phys. Rev. D 31 1323 (1985).
  • (12) P. Laguna-Castillo and R. A. Matzner, Phys. Rev. D 35 2933 (1987).
  • (13) A. Vilenkin and E.S. Shellard, Cosmic strings and other topological defects, Cambridge University Press (2000); M. Hindmarsh and T. Kibble, Cosmic strings, Rept. Prog. Phys. 58, 477 (1995).
  • (14) Planck Collaboration Collaboration, P. Ade et al., Planck 2013 result XXV. Searches for cosmic strings and other topological defects, [arXiv:1303.5085].
  • (15) See for instance, J. Polchinski, Proceedings of the NATO Advanced Study Institute and EC Summer School Cargese 2004, p.229-253, Dordrecht, Netherlands: Springer (2006); A. C. Davis and T. W. B. Kibble, Contemp. Phys. 46 313 (2005).
  • (16) E. Witten, Phys. Lett. B 153, 243 (1985).
  • (17) P. A. R. Ade et al. [BICEP2 Collaboration], Phys. Rev. Lett. 112 241101 (2014).
  • (18) J. Lizarraga, J. Urrestilla, D. Daverio, M. Hindmarsh, M. Kunz and A. R. Liddle, Phys. Rev. Lett. 112 171301 (2014).
  • (19) M. Majumdar and A. Christine-Davis, JHEP 0203 (2002) 056; S. Sarangi and S. H. H. Tye, Phys. Lett. B 536, 185 (2002); N. T. Jones, H. Stoica and S. H. H. Tye, Phys. Lett. B 563 6 (2003).
  • (20) R. Jeannerot, J. Rocher and M. Sakellariadou, Phys. Rev. D 68, 103514 (2003).
  • (21) N. Bevis et al, Phys. Rev. D75, 065015 (2007); N. Bevis et al, Phys. Rev. Lett. 100 021301 (2008); N. Bevis et al, Phys. Rev. D76, 043005 (2007); N. Bevis, M. Hindmarsh, M. Kunz and J. Urrestilla, Phys. Rev. Lett. 100, 021301 (2008); Phys. Rev. D 75, 065015 (2007); Phys. Rev. D 82, 065004 (2010); JCAP 1112, 021 (2011).
  • (22) J. Urrestilla, P. Mukherjee, A. R. Liddle, N. Bevis, M. Hindmarsh and M. Kunz, Phys. Rev. D 77, 123005 (2008); Phys. Rev. D 83, 043003 (2011).
  • (23) P. Saffin, JHEP 09, 011 (2005).
  • (24) B. Hartmann and J. Urrestilla, JHEP 07, 006 (2008).
  • (25) M. Christensen, A.L. Larsen and Y. Verbin, Phys. Rev. D 60, 125012 (1999).
  • (26) Y. Brihaye and M. Lubo, Phys. Rev. D 62 085004 (2000).
  • (27) U. Ascher, J. Christiansen and R. D. Russell, Math. Comput. 33 (1979), 659; ACM Trans. Math. Softw. 7 (1981), 209.
  • (28) E. Witten, Nucl. Phys. B 249, 557 (1985).
  • (29) P. Peter and J.-P. Uzan, Primordial Cosmology, Oxford University Press, 2009.
  • (30) B. Carter, Phys. Lett.B 228 466 (1989).
  • (31) B. Carter, in Formation and Evolution of Cosmic strings, edited by G. W. Gibbons, S. W. Hawking and T. Vachaspati, Cambridge University Press, 1990.
  • (32) P. Peter, Phys. Rev. D 45, 1091 (1992).
  • (33) B. Hartmann and F. Michel, Phys. Rev. D 86 105026 (2012).

Appendix A Appendix: the conservation law

In order to write down (6) explicitly we need the non-vanishing Christoffel symbols associated to the metric and in particular - since the energy-momentum tensor is diagonal - only the Christoffel symbols with equal lower indices. The non-vanishing Christoffel symbols with equal lower indices are

(40)

The conservation law (6) reads explicitly taking only the non-vanishing terms into account

(41)

Now using that and (40) we find

(42)

where the prime denotes the derivative with respect to . This can be rewritten in the following form

(43)

where we have sorted terms with respect to pre-factors of and , which are and respectively. This then leads to quasi-linear 2nd order differential equations in the fields and . Now, we require the respective terms in the brackets to vanish. This gives the equations (25) and (26). We believe that this is a suitable choice for our model. We insist that the model we are using here is phenomenological and as such our choice of equations is one possible choice amongst others. The use of phenomenological models to describe quantum effects in curved space-time is a widely used procedure since - up to now - a fully consistent model of quantum gravity does not exist.

Comments 0
Request Comment
You are adding the first comment!
How to quickly get a good reply:
  • Give credit where it’s due by listing out the positive aspects of a paper before getting into which changes should be made.
  • Be specific in your critique, and provide supporting evidence with appropriate references to substantiate general statements.
  • Your comment should inspire ideas to flow and help the author improves the paper.

The better we are at sharing our knowledge with each other, the faster we move forward.
""
The feedback must be of minimum 40 characters and the title a minimum of 5 characters
   
Add comment
Cancel
Loading ...
230701
This is a comment super asjknd jkasnjk adsnkj
Upvote
Downvote
""
The feedback must be of minumum 40 characters
The feedback must be of minumum 40 characters
Submit
Cancel

You are asking your first question!
How to quickly get a good answer:
  • Keep your question short and to the point
  • Check for grammar or spelling errors.
  • Phrase it like a question
Test
Test description