Running Inflation in the Standard Model

Running Inflation in the Standard Model

Andrea De Simone1,  Mark P. Hertzberg1,  and Frank Wilczek1
Center for Theoretical Physics and Department of Physics,
Massachusetts Institute of Technology, Cambridge, MA 02139, USA
11Electronic address: andreads at

An interacting scalar field with largish coupling to curvature can support a distinctive inflationary universe scenario. Previously this has been discussed for the Standard Model Higgs field, treated classically or in a leading log approximation. Here we investigate the quantum theory using renormalization group methods. In this model the running of both the effective Planck mass and the couplings is important. The cosmological predictions are consistent with existing WMAP5 data, with (for ) and negligible gravity waves. We find a relationship between the spectral index and the Higgs mass that is sharply varying for  GeV (depending on the top mass); in the future, that relationship could be tested against data from PLANCK and LHC. We also comment briefly on how similar dynamics might arise in more general settings, and discuss our assumptions from the effective field theory point of view.

Higgs Boson, Cosmological Inflation, Standard Model
14.80.Bn, 98.80.Cq
journal: Physics Letters B

1 Introduction

The hypothesis that there was a period in the early history of the universe during which a local Lorentz invariant energy density – i.e., an effective cosmological term – dominated the equation of state, causing exponential expansion, explains several otherwise puzzling features of the present universe (flatness, isotropy, homogeneity) Guth ; Linde ; AlbrechtSteinhardt82 ; Linde83 . It also suggests a mechanism whereby primordial density fluctuations arise through intrinsic fluctuations of quantum fields, leading to qualitative and semi-quantitative predictions that are consistent with recent observations. However the physics behind inflation remains mysterious. What, specifically, is the source of the energy density? Ideas ranging from fields associated with supersymmetry, string moduli, ghosts, branes, and others abound ModLinde ; ModLiddle ; ModDvali ; ModMcAllister ; ModNima ; ModKachru . One (or more) of them might be correct, but all are highly speculative, and none is obviously compelling.

Alternatively, we can look for inflationary dynamics based on degrees of freedom already present in the Standard Model. We can also attempt to maintain the guiding philosophy of the Standard Model, including gravity, to allow only local interactions which are gauge invariant and have mass dimension . Within this very restrictive framework, there remains the possibility to include the non-minimal gravitational coupling . Here is the Higgs field, is the Ricci scalar, and is a dimensionless coupling constant, whose value is unknown and largely unconstrained by experiment.444For the Higgs is conformally coupled to gravity. Indeed renormalization of the divergences arising in a self-interacting scalar theory in curved spacetime requires a term of this form BirrellDavies . The Higgs sector is then described, classically, by the Lagrangian


where is the Higgs self coupling and is the Higgs mass parameter.

It has been known for some time that such minimal classical Lagrangians can support inflation driven by an interesting interplay between the quartic term and the non-minimal coupling term Salopek ; Fakir ; Kaiser ; Komatsu . For ease of reference, we will call this general set-up “running inflation”; the name seems appropriate, since evolution of the effective Planck mass and the effective scalar mass is central to the dynamics.555The term “running inflation” was used in a different context in runningpaper . This quasi-renormalizable set-up allows use of renormalization group methods, as will be illustrated here. By quasi-renormalizable, we mean that the theory is renormalizable when gravity is treated classically; in particular, we ignore quantum corrections from graviton exchange (see Appendix B). In the investigation of (non-gravitational) quantum effects, it is appropriate to focus specifically on the Standard Model, for two reasons. First, because (as we will see) it illustrates important qualitative issues in a very concrete, familiar setting. Second, because it – or something close to it – might actually contain the degrees of freedom relevant to real-world inflation, in which case the specific predictions we derive could help describe reality.

Recently, the idea that the Standard Model Higgs field, non-minimally coupled to gravity, can lead to inflation was proposed in Ref. Bezrukov . Those authors argued that the radiative corrections to the potential are negligible and hence the inflationary parameters can be computed using the classical Lagrangian. They found that the cosmological predictions are in good agreement with cosmological data, independent of the Standard Model parameters, such as . On the other hand the authors of Ref. Barvinsky criticized their approach, suggesting that the quantum corrections to the potential can be very important. They concluded that a Higgs lighter than  GeV cannot serve as the inflaton, because the predicted spectral index is ruled out by WMAP5 data wmap5 . Ref. Barvinsky only incorporated quantum corrections at leading log order, extrapolated from low energies. Here, in contrast, we will compute the full renormalization group improved effective action at 2-loops. We conclude that running inflation based upon a Standard Model Higgs makes predictions that are consistent with current cosmological data, and leads to firm predictions for the PLANCK satellite and the LHC. Our main result is a correlation between the spectral index and the Higgs mass, see Fig. 1. This correlation is absent in the classical theory. The origin of the correlation lies in the interactions of the Standard Model, which dictate the form of the effective action.

In Section 2 we review inflation with non-minimally coupled scalars. In Section 3 we investigate the classical theory of the Higgs non-minimally coupled to gravity. In Section 4 we describe our method for obtaining the quantum corrected effective action. We compute all the inflationary observables numerically and present results in Section 5. Finally, we review our results and discuss their significance in Section 6.

Figure 1: The spectral index as a function of the Higgs mass for a range of light Higgs masses. The 3 curves correspond to 3 different values of the top mass:  GeV (red curve),  GeV (blue curve), and  GeV (orange curve). The solid curves are for , while for  GeV (blue curve) we have also indicated the 2-sigma spread in , where the dotted (dot-dashed) curve corresponds to smaller (larger) . The horizontal dashed green curve, with , is the classical result. The yellow rectangle indicates the expected accuracy of PLANCK in measuring () and the LHC in measuring ( GeV). In this plot we have set .

2 Non-Minimal Inflation

Here we briefly review the recipe to compute inflationary observables, which will be used in the later sections, and the latest observational constraints.

Consider a real scalar field non-minimally coupled to gravity via the Ricci scalar . The class of effective actions we consider is


where we allow for a general coefficient of the Ricci scalar , general coefficient of kinetic energy , and general potential . Here GeV is the reduced Planck mass; we are effectively assuming that the field is stabilized at the end of inflation with , as will be the case for the Standard Model Higgs.

The cosmology of this theory is most easily studied by performing a conformal transformation to the so-called “Einstein frame” where the gravity sector is canonical . This is achieved by defining the Einstein metric as . The corresponding Einstein frame potential is


Furthermore, the kinetic energy in the Einstein frame can be made canonical with respect to a new field , defined through the equation


(the second term here comes from transforming the Ricci scalar). In this frame, the action takes the canonical form


which is amenable to straightforward analysis.

The inflationary dynamics and cosmological predictions is determined by the shape of the potential . In the usual way, we introduce the first and second slow-roll parameters, which control the first and second derivatives of the potential, respectively. Using the chain rule, these are


where a prime denotes a derivative with respect to . Similarly, the third slow-roll parameter is related to the third derivative of the potential as .

The number of e-foldings of slow-roll inflation is given by an integral over :


where is the value of the field at the end of inflation, defined by . The number of e-foldings must be matched to the appropriate normalization of the data set and the cosmic history, with a typical value being ; we return to this point in Section 5.

The amplitude of density perturbations in -space is specified by the power spectrum:


where is the amplitude at some “pivot point” , predicted by inflation to be


and measured by WMAP5 to be at wmap5 . The corresponding spectral index , running of the spectral index , and tensor to scalar ratio , are given to good approximation by


The combined WMAP5 plus baryon-acoustic-oscillations (BAO) and supernovae (SN) data considerably constrain and . Assuming negligible , as will be the case for running inflation, the constraints are: and (at 95% confidence level).

3 Classical Analysis

Without essential loss we can rotate the Higgs doublet so that it takes the form . Only the real field will play a role in our analysis. Specializing to gauge invariant, dimension operators, without higher derivatives, the functions , , and must take the form


where GeV is the vacuum expectation value for the Higgs field, setting the electroweak scale. The self coupling is in one-to-one correspondence with the Higgs mass, namely . Current experimental bounds on the Higgs mass (and hence ) are as follows:


where the lower bound comes from direct searches and the upper bound comes from a global fit to precision electroweak data (95% CL) PDG .

In this theory, inflation takes place at energies many orders of magnitude above the electroweak scale (). Hence, during inflation the potential is well approximated by the quartic potential: , and this form of the classical potential will be sufficient throughout this Letter. The corresponding potential in the Einstein frame is then


which approaches a constant at large field values (we assume ). This fact allows slow-roll inflation to take place Salopek ; Kaiser ; Bezrukov . It is notable that through this mechanism slow-roll inflation emerges unusually “naturally”.

It is useful to define the dimensionless quantity which controls the cosmological evolution: inflationary stage (), the end of inflation (), and the low-energy regime (). Indeed the potential plotted in Fig. 2 displays the familiar quartic behavior for small values, but asymptotes to a constant for large .

Figure 2: The potential in the Einstein frame , normalized to a reference value , as a function of the Higgs field . The dashed green curve is the classical case (independent of Higgs mass), the solid blue (red) curve is the quantum case with Higgs mass  GeV ( GeV). We have set  GeV and for this plot. The inset focusses on the slow-roll inflationary regime.

Using eqs. (4), (6), and (7), the slow-roll parameters are readily computed. The exact results are not very transparent. They simplify for large , which is the case of physical interest:


We see that at large (during slow-roll inflation) is dominant, and will primarily control the predictions for the spectral index. The number of e-foldings is computed from eq. (8) giving


where is the value of at the end of inflation (). Eqs. (17) and (18) provide a parametric description of , , and , thus determining , , and as a function of , i.e., we can trade the unknown value of the Higgs field during inflation for the number of e-foldings .

For we find the following results for the spectral index, the running of the spectral index, and the tensor to scalar ratio:


We see that and are rather small. This will remain qualitatively true in the quantum theory, but the corrections to are quite important, as we explore in detail in the next section.

Finally, using eq. (10) and expanding to leading order in , the amplitude of density fluctuations is found to be


Since this must be , it is impossible to satisfy for and (which might be considered “natural” values). One possibility is that is extremely small, but that is incompatible with experimental bounds on the Higgs mass, see eq. (15), and is not stable under renormalization. Instead, following Bezrukov , we assume in order to obtain the correct amplitude of density fluctuations with . The need to dial a parameter to large or small values, so that is consistent with observations, is a common feature to all known inflation models. It will also apply in the quantum theory.

4 Quantum Analysis

We now consider how quantum corrections modify the classical results of the previous section. In order to do so, we need to compute the effective action that takes into account the effects of particles of the Standard Model interacting with the Higgs boson through quantum loops. The frame we calculate in is the original “Jordan” frame which defines the theory. The quantum theory modifies all three functions , , from the classical expressions in eq. (14).

The quantum corrections to the classical kinetic sector arise from wave-function renormalization, and are approximately –independent. It is simple to check that at large the second term in eq. (4) scales as , while the contribution from the term scales as . Hence corrections to occur with a factor , in addition to suppression by loop factors and couplings.

The quantum corrections to the classical gravity sector are more subtle. Let us start by considering the case of a (classical) background gravitational field. In this case the conformal anomaly induces a 1-loop -function for given by confbeta


The term proportional to , coming from Higgs running in a loop (see Fig. 3(a)), is potentially important during inflation. We will return to this point soon when we include the (classical) back reaction of gravity, and argue that in fact this contribution is negligible. The remaining terms arise from external leg corrections and cancel against wave-function renormalization to good approximation. Hence corrections to are ignorable also.

Figure 3: Some representative Feynman diagrams. Top row: renormalization of the conformal coupling with Higgs in loop (a), and renormalization of top quark’s Yukawa coupling with gauge boson (b) and Higgs (c) across vertex. Bottom row: renormalization of quartic coupling with Higgs (d), top quark (e), and gauge boson (f) in loop.

Finally we turn to the computation of the potential sector . Let us begin with the flat space analysis. The RG improved potential for the Higgs in the Standard Model is (see e.g. Ref. Sher for a review)


() where , and is the normalization point; taken to be in this Letter. Here encodes the running of , while , where is the anomalous dimension of the Higgs field, encodes wave-function renormalization. The running of is governed by the renormalization group equation: . At 1-loop it is


At low energies, the two most important terms here are the self coupling (see Fig. 3(d)), which tries to drive to large positive values, and the top quark (see Fig. 3(e)), which tries to drive towards zero. This is summarized in Fig. 4. This leads to a delicate interplay between the Higgs mass and the top mass. For , the term dominates and will eventually hit a Landau pole at high energies. For , the dominates and will go negative which is a sign of vacuum instability. The “Goldilocks” window for the Higgs mass, where the theory is both perturbative and stable up to very high energies is also the regime in which the quantum corrections are relatively small, allowing for slow-roll inflation. At high energies, the contribution from gauge bosons (see Fig. 3(f)) are important and increase .

Figure 4: This plot summarizes some of the most important effects of the renormalization group flow. The red curve shows the running of the quartic coupling for a light Higgs  GeV. The dotted purple curve is the top running and the dot-dashed cyan curve is the commutator function , with and . The right-hand region is the slow-roll inflationary regime; here rises (and so does too), as highlighted by the inset.

In the recent work of Barvinsky et al. Barvinsky the top quark’s Yukawa coupling was approximated by the tree level value: for all energy scales. This provides a significant negative contribution to , forcing to negative values and vacuum instability in large regions of parameter space. Instead it is essential to include the running of the top Yukawa coupling in the analysis:


which is negative due to the large negative contribution from the strong coupling (see Fig. 3(b)). Hence runs to smaller values at high energies; see Fig. 4.

In our work, we have included the complete running of the 5 couplings: , , , , and to 2 loops, to ensure accurate results.666The 3-loop running is unknown for the Standard Model, but would need to be abnormally large to have an effect. The -functions are summarized in Appendix A. Furthermore, we have adopted the pole mass matching scheme for the Higgs and top masses, given in the Appendix of Giudice . For the sake of brevity, we do not reproduce the pole matching details here.

We now consider the effective potential including the effect of the non-minimal coupling to gravity . The calculation is difficult to perform exactly. However, we can obtain approximate results for large fairly simply. Following Salopek , one can heuristically identify a non-standard commutator for as follows. From eqs. (4) and (5) we see that when the gravity sector is canonical, the kinetic sector is non-canonical On a spatial hypersurface, the canonical momentum corresponding to is


where is a unit timelike vector. Imposing standard commutation relations for and , we learn that , with


For (the low energy regime) we recover the ordinary value of the commutator , while for (the inflationary regime) we see a suppression in the commutator by a factor of . So in the inflationary regime with , quantum loops involving the Higgs field are heavily suppressed.

To summarize, our prescription for the renormalization group improved effective potential in the presence of non-minimal coupling is to assign one factor of for every off-shell Higgs that runs in a quantum loop. This factor is plotted as the dot-dashed cyan curve in Fig. 4. In eq. (23), for example, this prescription means the replacement , as that term arises from two Higgs off-shell propagators, while all other terms are untouched since they only involve other fields in loops (see Appendix A for more details). This provides an important modification to the high energy running of couplings, and explains why the running of from the diagram of Fig. 3(a) is suppressed. Apart from this modification, the RG improved analysis is as standard, as summarized in eq. (22). We have checked our prescription against detailed analytical calculations of the effective action of non-minimally coupled scalars in the literature (e.g., see Barvinsky2 ; Barvinsky3 ) and have found excellent agreement. We assume that quantum corrections from graviton exchange are small, see Appendix B.

5 Results and Predictions

After numerically solving the set of 5 coupled renormalization group differential equations of Appendix A for the couplings: , , , , and , we have obtained the effective potential in the full quantum theory, as a function of input parameters, such as the Higgs mass. Some representative potentials in the Einstein frame are given in Fig. (2). The inset clearly exhibits variation of the effective potential with Higgs mass, which was absent in classical case. As we lower the Higgs mass, approaching the instability, the magnitude of the first derivative is raised and the that of the second is lowered (see the blue and red curves). This leads to modifications to the cosmological parameters.

Following the recipe we outlined earlier in Section 2, we are able to efficiently compute the spectral index in the RG improved theory using Mathematica. Recall that in the classical theory, is independent of the parameters of the Standard Model, and its value was found to be (for ). In the quantum theory, we find that depends on several of the Standard Model parameters, in particular on the Higgs and top masses, see Fig. 1. As the top mass is varied through its experimentally allowed range (GeV) the spectral index varies noticeably. In particular, as we lower the Higgs mass towards vacuum instability, the spectral index increases substantially. To achieve successful inflation with , we require


where  GeV indicates theoretical uncertainty from higher order corrections (such as 3-loop). This bound almost coincides with that from absolute stability presented in Ref. Giudice . Note that near the boundary is small, so the corresponding to obtain the observed is reduced from its classical value by an order of magnitude or so to .

Let us now trace the chain of logic behind the rise in . For a light Higgs, is dominated by the top and gauge boson contributions. For a heavy top, the top contribution is dominant at low energies, causing to be negative and thus driving to low values as the energy is increased. At the same time, the top Yukawa coupling runs, with dominant contributions coming from gauge fields and Higgs running in a loop, with the gauge fields slightly dominant causing to decrease with energy.777Note that the 2-loop term in (see eq. (34)) speeds up the running compared to 1-loop. At very high energies (the inflationary regime), the Higgs running in the loop is highly suppressed, causing to jump to even lower values. Hence the top contribution to the running of becomes subdominant, the gauge boson contributions now dominate and rises, as seen in Fig. 4 (inset). Since is concave up, this increases and hence the spectral index.

In Fig. 1 and in all plots we have chosen the reference value . For close to , we can Taylor expand to linear order:


Now, the spectral index is in fact a function of all the parameters, including and : . As in the classical theory, we have fixed such that the amplitude of density fluctuations is in agreement with observations (requiring ). In this way, we can think of , so from the chain rule


The first term is precisely the (negative) of the running of the spectral index , while the second term is found to be very small numerically. Hence to a good approximation we can write


We plot the running of the spectral index in Fig. 5 (left). We see that (as in the classical case), with some variation for low Higgs masses as we approach the instability. However, this is still far too small to be detected by PLANCK, which is expected to be only sensitive to Liddlerunning . Hence the main usefulness of Fig. 5 (left) is that it should be used in accompaniment with Fig. 1 and eq. (30) to infer the value of for different values (as long as does not vary too far from ).

Figure 5: The running of the spectral index (left panel) and the tensor to scalar ratio (right panel) as a function of the Higgs mass . The 3 solid curves correspond to 3 different values of the top mass:  GeV (red curve),  GeV (blue curve), and  GeV (orange curve). The horizontal dashed green curve, with and , is the classical result. We have set and in this plot.

The actual number of e-foldings of inflation is related to the wavenumber of interest , the energy density during inflation , the energy density at the end of inflation , and the energy density at the end of reheating ModLiddle


Since the Higgs is strongly coupled to Standard Model fields, reheating is expected to occur automatically. As has only a weak dependence on , the details of reheating are rather inconsequential to our mass bounds, but may be calculable Bellido . According to Bezrukov2 ,  GeV giving for the classical theory. In our case, we must take into account the variation in the scale of inflation due to the quantum corrections. In Fig. 5 (right) we plot versus the Higgs mass. Since we have fixed such that the amplitude of density fluctuations is at the observed value, the energy density of inflation is simply proportional to . Using eqs. (10) and (13), we have


Since changes by a factor of order 2, as we vary the Higgs mass, then changes by the same amount. From eq. (31), rescaling and by a factor of , say, the number of e-foldings is shifted by , which is for . Hence the variation in with the Higgs mass is very small.

6 Discussion

A number of papers have discussed bounds on the Higgs mass coming from demanding stability of the vacuum, e.g., see Sher ; Giudice ; Nimabds ; Isidori . Cosmological constraints only require metastability on the lifetime of the universe, which places the constraint  GeV Giudice . However, if we further demand that the Higgs drive inflation, we find that heavier Higgs are required:  GeV (depending on the top mass, see eq. (27)), which essentially coincides with the bounds from absolute stability. Furthermore, by demanding that the theory remains perturbative to high energies ( GeV), we establish a correlation between both stability and triviality bounds, and inflation.

More precisely, we have established a mapping between the renormalization group flow and the cosmological spectral index. Over a substantial range of parameter space the classical value (for ) emerges as a good approximation, but there are corrections. Given a detailed microphysical theory, such as the Standard Model, we can explicitly calculate such corrections, as summarized in Fig. 1. This plot displays a sharp rise in the spectral index towards 0.98, or so, as we approach vacuum instability for a light Higgs.

It is likely that the Standard Model is only the low-energy limit of a more complete theory, accommodating the facts that do not find explanation within the Standard Model, such as neutrino masses, dark matter, baryon asymmetry, etc. Our methodology is still applicable, so long as we can control the relevant -functions.

In principle some quite different scalar field, not connected to the Standard Model Higgs, could drive running inflation. The central requirement is a large coefficient for the term. It is possible that such a coefficient could emerge as some sort of Clebsch-Gordan coefficient, or from the coherent addition of several smaller terms (involving more basic scalars ). It is also possible to consider, in the same spirit, the dimension 3 interaction , which arises for generic scalar fields, though not of course for the Standard Model Higgs. Furthermore, as discussed in Appendix B and Refs. Burgess ; Espinosa , the inclusion of higher dimension operators may significantly affect the predictions of the original theory and even spoil its validity (as is the case in many inflationary models). These possibilities, and their possible embedding in unified field theory or string theory, deserve further investigation.

If the Higgs boson exists and it is in the mass range considered in this Letter, the LHC will discover it and will determine the Higgs mass with a precision of about tdr , which means an uncertainty GeV. In order to extract accurate correlations between the inflationary observables and the Higgs mass it is crucial to improve the precision with which we know the other parameters of the Standard Model, in particular the top quark mass and the strong coupling. The current value of the top mass from direct observation of events is GeV PDG . In the near future, the LHC will improve the determination of the top mass, but relatively large systematic uncertainties will prevent a top mass determination to better than GeV; more conservatively, the top mass will be determined at LHC with an error GeV. Looking further ahead, the ILC is expected to be able to measure the top mass to  MeV. So together with the measured Higgs mass from the LHC and improved precision on the strong coupling, as well as calculating higher order effects and reheating details, running inflation in the Standard Model will predict a rather precise value for the spectral index.

We would like to thank M. Amin, F. D’ Eramo, A. Guth, and C. Santana for useful discussions, and A. Riotto for comments on the manuscript. We thank F. L. Bezrukov, A. Magnin, and M. Shaposhnikov for correspondence. The work of ADS is supported in part by the INFN “Bruno Rossi” Fellowship. The work of ADS, MPH, and FW is supported in part by the U.S. Department of Energy (DoE) under contract No. DE-FG02-05ER41360.

Note Added

Our Letter appeared simultaneously on the arXiv with Ref. Bez2008 , which also studied the quantum corrections to inflation driven by the Standard Model Higgs. The central conclusion of both papers is that the classical analysis provides a good approximation over a wide range of parameters, but that quantum corrections are calculable and can be quantitatively significant.

For a top mass of  GeV, Ref. Bez2008 found that in order to have successful inflation the Higgs mass is constrained to be in the range: , and the spectral index decreases from its classical value as approaches the lower boundary. In this note we briefly discuss the similarities and differences between their analysis and ours.888The discussion here refers to version 1 of Bez2008 .

In our analysis, we computed the full RG improved effective potential. We did this including (i) 2-loop beta functions, (ii) the effect of curvature in the RG equations (through the function ), (iii) wave-function renormalization, and (iv) accurate specification of the initial conditions through proper pole matching. On the other hand, Bez2008 did not compute the full effective potential or include any of the items (i)–(iv).999Though wave-function renormalization was not included in Bez2008 , external leg corrections in the running of were included. However these two effects roughly cancel against one another. Instead Ref. Bez2008 approximated the potential at leading log order with couplings evaluated at an inflationary scale after running them at 1-loop (this is one step beyond Barvinsky where couplings were not run).

The lower bound on the Higgs mass we find in eq. (27) is about 11 GeV lower than that found in Ref. Bez2008 ( GeV). This numerical discrepancy is due to several of the above simplifications, but the dominant difference comes from (i) inclusion or not of 2-loop effects (importantly, the term in , see eq. (34)), and a second significant difference comes from (iv) pole matching. Higher order effects (such as 3-loop) and uncertainty in the strong coupling also modify the bound, as we summarized in eq. (27).

A precise upper bound on the Higgs mass ( GeV) is stated in Bez2008 . The basis of this is the famous “triviality bound”, see e.g., Ref. Ellis , which has little to do with inflation. The theory ultimately requires a cutoff, and exactly how low a cutoff one feels comfortable with (or equivalently, how large a value of one regards as acceptable) is arguable. We feel that our stated semi-quantitative bound  GeV adequately represents the situation.

In Bez2008 decreases as approaches its minimum value, while we find that increases (see Fig. 1). This behavior depends critically on the value of during inflation, as compared to the value of the gauge couplings. If is small, then increases, and vice versa. Ref. Bez2008 overestimated during inflation and hence obtained the opposite behavior. This is primarily due to ignoring items (i) and (ii) above. Ignoring (i) misses the 2-loop term in , and ignoring (ii) maintains the 1-loop term in during inflation.

Finally, Bez2008 computes quantum corrections with both a field-independent cutoff (as we use) and a field-dependent cutoff in the original “Jordan” frame. Either procedure defines a possible model, but the field-independent cutoff is more in the spirit of the motivating arguments, based on dimension effective Lagrangians.

Appendix A 2-Loop RG Equations

In this appendix we list the RG equations for the couplings at energies above at 2-loop Ford . In each case, we write , etc., where . Also, we insert one factor of the commutator function (see eq. (26)) for each off-shell Higgs propagator.101010We have carefully extracted out all Higgs propagators contributions at 1-loop order by the appropriate insertion of factors of . For the 2-loop contributions we have only inserted for the obvious terms. The complete set of insertions are tedious and provide negligible corrections.

For the Higgs quartic coupling we have


For the top Yukawa coupling we have


For the gauge couplings we have




Finally, the anomalous dimension of the Higgs field is


Appendix B Remarks on Running Inflation as an EFT

The Lagrangian analyzed in this Letter is not renormalizable in the conventional sense, nor is it “technically natural” from the point of view of effective field theory. In this appendix we remark on the validity of such a theory at high energies (for related discussions see Burgess ; Espinosa ) and elaborate on the spirit of our calculations.

The novelty of running inflation is to introduce the non-minimal coupling into the low energy Lagrangian, which is allowed by all known symmetries of the Standard Model and gravity. This term is dimension 4 in the same sense that the kinetic term is also. However, if we expand around flat space then the new term is dimension 5 at leading order, plus an infinite tower of corrections

which is connected to the non-renormalizability of gravity in 4 dimensions. This suggests that non-minimally coupled theories becomes strongly interacting at scales . This can be compared to minimally coupled theories with .

Without any protecting symmetry, we cannot forbid infinite towers of corrections to the dimension 4 effective Lagrangian , including those of the form

which applies to non-minimal models (with ) and minimal models (with ). The values of the higher order Wilson coefficients cannot be determined without knowledge of the behavior of gravity at energy scales above , since these terms arise from graviton exchange. If we take a naive estimate , then the required flatness of the inflationary potential is jeopardized. This applies both to running inflation and to many minimal inflation models, such as chaotic inflation, since in both cases during inflation. As there is no increased symmetry in the limit , such theories are not “technically natural”.

On the other hand, we currently have no evidence for , as these terms arise from graviton exchange, whose effects are yet to be seen in any experiment. There does exist a logical possibility that graviton exchange at high scales is softer than naive estimates suggest (Ref. Horava may be an example), rendering small, preserving unitarity, and leaving our calculated potential essentially unaltered. It is in this spirit of including only the known Standard Model loops, and not those of unknown graviton loops, that we have obtained our results and predictions – which are highly falsifiable.


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
Loading ...
This is a comment super asjknd jkasnjk adsnkj
The feedback must be of minumum 40 characters
The feedback must be of minumum 40 characters

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 description