_{1}

^{*}

Cosmic inflation is considered assuming a cosmologically varying Newtonian gravitational constant,
*G.* Utilizing two specific models for,
*G*
^{-1}(a), where, a, is the cosmic scale parameter, we find that the Hubble parameter,
*H*, at inception of
*G*
^{-1}, may be as high as 7.56 E53 km/(s Mpc) for model A, or, 8.55 E53 km/(s Mpc) for model B, making these good candidates for inflation. The Hubble parameter is inextricably linked to
*G* by Friedmanns’ equation, and if
*G* did not exist prior to an inception temperature, then neither did expansion. The CBR temperatures at inception of
*G*
^{-1} are estimated to equal, 6.20 E21 Kelvin for model A, and 7.01 E21 for model B, somewhat lower than CBR temperatures usually associated with inflation. These temperatures would fix the size of Lemaitre universe in the vicinity of 3% of the Earths’ radius at the beginning of expansion, thus avoiding a singularity, as is the case in the ΛCDM model. In the later universe, a variable
* G *model cannot be dismissed based on SNIa events. In fact, there is now some compelling astronomical evidence, using rise times and luminosity, which we discuss, where it could be argued that SNIa events can only be used as good standard candles if a variation in
*G* is taken into account. Dark energy may have more to do with a weakening
*G* with increasing cosmological time, versus an unanticipated acceleration of the universe, in the late stage of cosmic evolution.

The Friedman equations and the ΛCDM model both assume that Newton’s constant, G, is a true constant of nature. Recently [

In reference [

Inflation is a theory [

In this paper, we argue for a different interpretation, one incorporating a variation in G with respect to cosmological time. In reference [

M P l = ( ℏ c / G ) 1 / 2 (1-1)

We square this result, and claim moreover, that G − 1 is an order parameter, satisfying,

M P l 2 = ℏ c G − 1 = 〈 0 | φ 2 | 0 〉 (1-2)

Here, the, M P l 2 , is no longer a constant, but the vacuum expectation value (VEV) of a scalar field, φ , squared. As the scalar field, φ , freezes out of the vacuum, G − 1 changes its value, a process lasting eons. In our scenario, G − 1 is no longer a constant, and neither is the Planck mass. We identify the scalar field in Equation (1-2), with the scalar field of Jordan, first introduced in 1937, but largely ignored when discussing inflation.

It should be noted that M P l 2 has the same canonical dimensions as magnetization in condensed matter physics, or M W ± 2 in particle physics. In the electro-weak interaction, M W ± , is the mass of the W ± boson. Thus, it could very well be an order parameter based on inherent dimension alone. It is well known that M W ± 2 is essentially the inverse Fermi constant, G F − 1 , which fades at high energies, and is only constant well below 100 GeV. Newton’s constant, and the Fermi constant, are the only two known coupling constants in physics, which have an inherent dimension, and that canonical dimension is the same for both. It can be expressed as inverse mass squared.

Model A, assumes [

G − 1 ( T ) = G ∞ − 1 ( 1 − e b / T ) (model A) (1-3)

In this equation, T is the temperature of the universe and G ∞ − 1 is a saturation value, achieved in the limit where, T → 0 . The constant “b” has units of temperature, but is independent of temperature. In model A, the constant, b, equals, b = 11.663 , which was determined by demanding that, w = − 0.98 . Also, G ∞ − 1 = 1.014 G 0 − 1 , where G 0 is Newton’s constant. In the current epoch we have the well-known, G 0 = 6.674 E − 11 , in MKS units. All units, which are not explicitly written out in this paper, are MKS units. The cosmic scale parameter, “a”, can be expressed as, a = ( 1 + z ) − 1 = T 0 / T = R / R 0 , where T is the CBR temperature, and in the present epoch, T 0 = 2.725 Kelvin . Using this relation, Equation (1-3), can be rewritten as,

G − 1 ( T ) = G ∞ − 1 ( 1 − e − 4.28 a ) (model A) (1-4)

This equation came into being at a temperature estimated [

Model B, assumes an entirely different scaling law, namely,

G − 1 ( T ) = G ∞ − 1 [ coth ( b / T ) − T / b ] (model B) (1-5)

Again, G ∞ − 1 is the saturated value, applicable in the limit where the CBR temperature, T → 0 . We could just as well have called, G ∞ − 1 = G T = 0 − 1 . The constant, “b”, having units of Kelvin, has been determined to equal, b = 48.15 Kelvin , in order to guarantee that the quintessence parameter, w = − 0.98 . Again, the parameter, “b”, per se, is independent of CBR temperature, even though it is measured in units of Kelvin. Here, in model B, it is found that, G ∞ − 1 = 1.054 G 0 − 1 .

The nonlinear function, Equation (1-5), is recognized as the Langevin function, defined as, L ( x ) ≡ coth ( x ) − 1 / x , used in magnetism. This is another approach towards modeling, G − 1 ( a ) , and we call this model B. The quantity, G − 1 ( a ) , has inherent canonical dimension of magnetization. Referring to equation (1-2), we treat 〈 0 | φ 2 | 0 〉 as an order parameter, much like magnetization. In terms of canonical dimension, magnetization has the same units as inverse mass squared, or inverse momentum squared.

Another way to rewrite Equation (1-5), is to remember that, a = ( 1 + z ) − 1 = T 0 / T = R / R 0 , where z is the redshift, and R, the Hubble radius. The temperature, T 0 = 2.725 , is the current CBR temperature. We substitute “a” in place of temperature, using the above expression for, “a”. In Equation (1-5), this gives,

G − 1 ( a ) = G ∞ − 1 [ coth ( 17.67 a ) − 1 / ( 17.67 a ) ] (model B) (1-6)

This order parameter surfaced [

In model B, the current value for Newton’s constant, G 0 , is not far from the final saturation value. In fact, we have the relation, G ∞ − 1 = 1.054 G 0 − 1 . Saturation in model B, will effectively occur at a CBR temperature, roughly half the present temperature of, 2.725 Kelvin. The universe will then have expanded its Hubble radius to twice its present value.

When plotted separately as a function of “a”, the scale parameter, both model A, and, model B, functions look very similar. At inception, G − 1 , will rise very dramatically from zero. This is because, at very high temperatures, the G − 1 is proportional to inverse temperature, T − 1 , in both models. As the CBR temperature decreases upon expansion, G − 1 will start to level off, and eventually start approaching a saturation value, indicated by, G ∞ − 1 . Currently, in the present epoch, we are close to saturation and that is the reason why G ˙ / G is very nearly equal to zero. In the current epoch, G ˙ / G is of the order, 10E−12 per year, a very small value.

Both models A and B, indicate inception temperatures of, 6.20E21 Kelvin, and, 7.01E21 Kelvin, respectively. Since G − 1 did not really exist prior to that point in cosmological time, neither did, G. And, in the simplest form of the Friedmann equation,

H 2 = 8 π G ρ / 3 (1-7)

this would indicate that the universe was not expanding at all until the temperature dropped down to the inception temperature. What existed beforehand, or what caused the universe to suddenly expand, is unknown. But as to what happened shortly thereafter, we have an idea given these two models for, G − 1 .

It turns out that using Equations (1-3), and (1-5), we can find the values of G at inception. Let G C = G ( T C ) where, T C is the Curie temperature. Then using the inception temperatures listed above, we find,

G C / G 0 = 5.27 E 20 (model A) (1-8a)

G C / G 0 = 4.11 E 20 (model B) (1-8b)

The high G C / G 0 values, indicated by Equations (1-8a, b), were needed to explain the cosmological constant problem, as shown in reference [

We next wish to find the corresponding Hubble parameter values at inception of, G − 1 . We will use Equation (1-7). The H C values would indicate the rate of expansion at roughly, 10E21 Kelvin. To determine, H C , we first need to estimate the mass/energy density, ρ C , at these very high temperatures. At temperatures of the order, 10E21 Kelvin, no elementary particles have yet condensed out of the vacuum. All quarks and leptons, i.e., all matter particles in the standard model, only froze out at lessor temperatures, below 10E16 Kelvin or approximately, 1 TeV [

ρ C = a C − 4 ( 8.3 E − 5 ) ( 8.624 E − 27 ) (1-9)

This, however, is only part of the story, because we have not taken into account the masses of the known elementary particles. When their flavors, and their degrees of freedom, are taken into account, we should properly multiply Equation (1-9), by a correction factor, g * = 106.75 . See references [

What remains is to find a C . But this is easy since we know the temperatures at inception, and, a C = T 0 / T C . For models A, and B, we find, respectively, that

a C = T 0 / T C = 4.40 E − 22 (model A) (1-10a)

a C = T 0 / T C = 3.89 E − 22 (model B) (1-10b)

These values are very close to one other because the inception temperatures were nearly equal. We next substitute these cosmic scale factors into Equation (1-9), and multiply the result by the correction factor, g * = 106.75 , to take masses, which were frozen out below 1 TeV, into account. The results are, respectively,

ρ Radiation , C = ρ Radiation ( T C ) = 2.04 E 57 (model A) (1-11a)

ρ Radiation , C = ρ Radiation ( T C ) = 3.34 E 57 (model B) (1-11b)

These are the values, which we will substitute into Equation (1-7). Keep in mind that Newton’s constant gets replaced by a new value, G C , when we do that. Those values are given by Equations (1-8a), and (1-8b), respectively.

We do this next. We substitute Equations (1-11a, b), and (1-8a, b), into Equation (1-7), and find, respectively, that the Hubble parameter equals

H C = 2.45 E 34 seconds − 1 (model A) (1-12a)

H C = 2.77 E 34 seconds − 1 (model B) (1-12b)

In MKS units, the Hubble parameter is measured in inverse seconds. Converting to the more standard, km/(s∙Mpc), we obtain,

H C = 7.56 E 53 km / ( s ⋅ Mpc ) (model A) (1-13a)

H C = 8.55 E 53 km / ( s ⋅ Mpc ) (model B) (1-13b)

Needless to say, these expansion rates are dramatic, especially in light of the fact that the current value of H 0 equals a mere 67.74 km/(s∙Mpc). Our view is that these high values indicate inflation. The so-called inflaton field, usually associated with inflation, will be replaced by a scalar field, φ , first introduced by Jordan in 1937, and highlighted in Equation (1-2). Equations (1-13a) or (1-13b), is our version of inflation.

As mentioned, what happens before this point in cosmological time is anyone’s guess. How the CBR temperature dropped down to, 10E21 Kelvin, in the first place if the universe didn’t expand prior to that point, is also a mystery. Interestingly, when Lemaitre first introduced his expanding universe hypothesis in the mid 1920’s, he never claimed that it evolved from a singularity. In fact, early critics derided his hypothesis by referring to it as his “cosmic egg” hypothesis [

The finite size can be estimated at the start of expansion. Since, a = R / R 0 = T 0 / T , we can set, R C = a C R 0 . Using a currently accepted estimate [

R C = a C R 0 = 1.94 E 5 meters (model A) (1-14a)

R C = a C R 0 = 1.71 E 5 meters (model B) (1-14b)

This is roughly 3 percent of the earth’s radius. This would be our initial estimate for the size of Lemaitre’s cosmic egg at the beginning of expansion.

We now turn to the later stages of cosmic evolution where we have dark energy. We want to consider, specifically, the increased luminosity distance associated with SNIa events, which led one to conclude that the universe is currently expanding more rapidly, than anticipated.

Consider a specific SNIa event, where the energy flux, measured on earth bound satellites, fixes a specific distance to the source using the luminosity-distance-flux relation. SNIa events, i.e., explosions, make for good standard candles because of their brightness, and excellent predictable luminosity. The observed distances, measured in the late 1990’s, and after, suggest that the universe is expanding faster than we thought. We have an unanticipated acceleration leading one to surmise, erroneously we believe, that in the later stages of cosmic evolution, a type of antigravity or negative pressure surfaces, which we identify as dark energy. What happens however, if G varies cosmologically?

The luminosity of a SNIa event varies as G − 3 / 2 [

Taking this a step further, we know that the energy flux received by an observer here on earth is related to the luminosity distance by the relation, Φ = L / ( 4 π d L 2 ) , where Φ is the flux, d L , the luminosity distance, and, L, the luminosity. Thus, if d L seems to increase unexpectedly, it may actually be due to L decreasing if one goes back in cosmological time. At higher redshifts, the luminosity, L, could be weaker. Let L 0 be the luminosity in the present epoch, and set d L equal to the expected distance without dark energy. Then the observed flux gives,

L 0 / d ′ L 2 = L / d L 2 = ( G / G 0 ) − 3 / 2 L 0 / d L 2 (2-1)

In this equation, d ′ L is the perceived and un-anticipated, accelerated luminosity distance, leading to the notion of dark energy. By contrast, d L , is the true luminosity distance. The increase in d ′ L over d L is really due to a decrease in G − 1 if one goes back in time. Equation, (2-1), can namely be rewritten as

d ′ L / d L = ( G / G 0 ) 3 / 4 (2-2)

It is apparent by this equation, that if G increases, then, d ′ L also increases. Depending on the look-back time, at a specific redshift, the G is stronger in value, and thus by Equation (2-2), this makes the ratio, d ′ L / d L , larger.

Models A, and B, for G = G ( a ) = G ( z ) , introduced in the last section, can now be substituted for the right hand side of Equation (2-2). We can predict the amount of unanticipated luminosity distance as a function of redshift since, a = ( 1 + z ) − 1 . Antigravity, or negative pressure, we argue, is caused by a declining G value as cosmological time advances. Or, if we go back in time, we obtain a larger d ′ L value.

As specific examples of accelerated expansion, we calculate ( G / G 0 ) at a redshift of, z = 1 / 2 , and then again, at, z = 2 / 3 . First, consider, z = 1 / 2 . Since, a = ( 1 + z ) − 1 , this corresponds to a = 2 / 3 . Equation, (1-4), model A, gives

G / G 0 = G 0 − 1 / G − 1 = [ 1 − e − 4.28 ] / [ 1 − e − ( 4.28 × 2 / 3 ) ] = 1.0465 (model A) (2-3)

Substituting this into Equation (2-2), we obtain

d ′ L / d L = 1.035 ( z = 1 / 2 , model A) (2-4)

For model B, we use Equation (1-6). Here,

G / G 0 = G 0 − 1 / G − 1 = [ coth ( 17.67 ) − 1 / 17.67 ] / [ coth ( 17.67 × 2 / 3 ) − 3 / ( 17.67 × 2 ) ] = 1.031 (model B) (2-5)

And therefore, by Equation (2-2), we expect,

d ′ L / d L = 1.023 ( z = 1 / 2 , model B) (2-6)

We emphasize that both functions, Equation (1-4), and Equation (1-6), for G − 1 ( a ) , are nonlinear.

Let us now carry out the same analysis for one further redshift. We now consider a redshift, z = 2 / 3 , or, a = ( 1 + 2 / 3 ) − 1 = 0.6 . Following the same steps as before, but for this new redshift, we obtain for model A,

d ′ L / d L = 1.051 ( z = 2 / 3 , model A) (2-7)

For model B, this ratio becomes,

d ′ L / d L = 1.036 ( z = 2 / 3 , model B) (2-8)

We have a clear increase in luminosity distance in Equations (2-7), and (2-8), when they are compared to Equations (2-4), and (2-6), respectively. We also notice that model, A, is more aggressive than model B, in predicting increases in, d ′ L / d L , at a specific z value.

There is some astronomical evidence that higher redshifted SNIa luminosities are weaker. Thorsett [

Not only is luminosity affected by Newton’s constant G, but also, τ , the rise and fall time, for SNIa events [

In summary, a G − 3 / 2 behavior for luminosity, and a G − 3 / 4 behavior for light curve widths, cannot be dismissed in a variable G model. SNIa events may not be the good standard candles we take them for, unless a variation in G is taken into account. Our models, A, and B, attempt to do just that, i.e., make reasonable predictions for d ′ L / d L given a specific redshift.

Cosmic inflation, i.e., the rapid expansion of the universe in its earliest phase, has been considered assuming a cosmologically varying G. The Friedmann equation, in particular, is invoked to argue that Hubble expansion is only possible if G is unequal to zero. If G varies with cosmological time, then it must be an intrinsic property of the vacuum. Moreover, it must be related to a scalar field, φ , as first suggested by Jordan. The Planck mass squared, M P l 2 , is no longer a constant, but related to φ 2 , as shown explicitly in Equation (1-2). The φ may also be interpreted as a new type of inflaton field, one associated with a time varying G, surfacing at a temperature we estimate to be about 10E22 Kelvin.

Two models for a time varying G − 1 were presented, models A, and B, given by Equations (1-4) and (1-6), respectively. Both functions rise dramatically at their respective inception temperatures, 6.20E21 Kelvin for model A, and 7.01E21 Kelvin for model B. In fact, at about these temperatures, both models give a G − 1 value, which is proportional to, 1/T, where T is the CBR temperature. The cosmological scale parameter, “a”, is related to CBR temperature by way of the equation, a = T 0 / T = ( 1 + z ) − 1 . Eventually, as the universe cools upon expansion, G − 1 levels and tapers off and approaches a saturation value, a constant in the limit where, a → ∞ .

There are only two coupling constants in nature, which have an inherent canonical dimension. The first is the Fermi constant, G F , in the theory of weak interactions. We now know that, in reduced units, G F − 1 is essentially equal to, M W ± 2 , where, M W ± is the mass of the W ± boson. This is at low energies. At high energies, above 100 GeV, the G F value increases. The second coupling constant with inherent canonical dimension is Newton’s constant. In fact, it has exactly the same canonical dimension as, G F . If we replace the mass of the W ± boson squared by the Planck mass squared, then we have an entirely analogous situation with regards to gravity. Keep in mind that the theory of weak interactions, in itself, is not renormalizable at high energies. It is only the broader electro-weak interaction, which is consistent at high energy/momentum transfers or exchanges. We believe that a similar situation holds for gravity. The Fermi constant, G F , is definitely an order parameter. At very high temperatures, the mass of the W ± boson becomes relatively unimportant, and we have, G F − 1 ~ ( p 2 − M W ± 2 ) approaching zero. The, p μ , is the momentum, of the mediating boson. At low temperatures, G F − 1 ~ M W ± 2 reduces to a constant. We believe the same scenario holds true for gravity and Newton’s constant, just at a much higher threshold temperature of approximately, 10E22 Kelvin.

Using our two models for, G − 1 ( a ) , we predict very high values for the Hubble parameter, at inception of G − 1 . The values, which were obtained, were given by equations, (1-12a, b), and (1-13a, b). We believe that these expansion rates could be interpreted as inflation, where the “inflaton” field of inflation is replaced by Jordan’s scalar field, φ , above. Beyond this point, temperature-wise, G, simply did not exist, and there was no expansion of space, as determined by the Friedmann equation. It is hypothesized that when the universe started to expand, it had a finite size, of the order of the earth’s radius. In the ΛCDM model, expansion started from a singularity.

Finally, a variable G model cannot be dismissed based on SNIa events. In fact, there is now some very solid observational/astronomical evidence indicating otherwise. A variable G may be needed to interpret SNIa energy release properly, as well as rise and fall times for these events. See Equations (2-1) and (2-2). Specific predictions for luminosity distance are possible using our two models for, G − 1 ( a ) , models A, and B. As specific examples, Equations (2-4) and (2-6), are results that apply for z = 1 / 2 . And for a larger redshift, z = 2 / 3 , we obtain Equations (2-7) and (2-8). It may well turn out that SNIa events, in order to serve as good standard candles, need to include a variation in Newton’s constant, G. Without taking into account a weakening G with an increase in cosmological time, erroneous results and interpretations occur. Dark energy may have more to do with a weakening in G with decreased redshift, than anything else.

The author would like to thank his children, Kira, Juergen, and Henry for simply being who they are.

The author declares no conflicts of interest regarding the publication of this paper.

Pilot, C. (2020) Inflation and Rapid Expansion in a Variable G Model. International Journal of Astronomy and Astrophysics, 10, 334-345. https://doi.org/10.4236/ijaa.2020.104018