A note on the cosmological constant in f(R) gravity

TL;DR

This paper examines the constraints on f(R) modified gravity models in cosmology, concluding that either Einstein's cosmological constant is necessary or dark energy's equation of state is more complex than a simple perfect fluid.

Contribution

It highlights the limitations of f(R) gravity in explaining late-time acceleration without reverting to Einstein's cosmological constant or complex dark energy models.

Findings

Einstein's cosmological constant remains the simplest explanation.

f(R) models must closely mimic Einstein gravity to fit observations.

Dark energy may not be well-described by a constant equation of state.

Abstract

The starting point in this note is $f(R)$ modified gravity in a cosmological setting. We assume a spatially flat Universe to describe late-time cosmology and the perfect-fluid equation of state $p=\omega\rho$ to model the hypothesized dark energy. Given that on a cosmological scale, $f(R)$ modified gravity must remain close to Einstein gravity to be consistent with observation, it was concluded that either (1) Einstein's cosmological constant is the only acceptable model for the accelerated expansion or (2) that the equation of state for dark energy is far more complicated than the perfect-fluid model and may even exclude a constant $\omega$.

Equations

$$S_{\text{EH}}=\int \sqrt{-g}R{d}^{4}x$$

$$S_{f(R)}=\int \sqrt{-g}f(R)d^{4}x.$$

$$\frac{\stackrel{..}{a}(t)}{a(t)}=-\frac{4\pi }{3}(\rho +3p).$$

$$d{s}^2=-e^{2\Phi (r)}d{t}^2+\frac{d{r}^2}{1-b(r)/r}+r^2(d{\theta }^2+{\text{sin}}^2\theta d{\varphi }^2).$$

$$\rho (r)=F(r)\frac{b^{\prime }(r)}{r^2},$$

$$p_r(r)=-F(r)\frac{b(r)}{r^3}+F^{\prime }(r)\frac{r{b}^{\prime }(r)-b(r)}{2r^2}-F^{\prime \prime }(r)\left(1-\frac{b(r)}{r}\right),$$

$$p_t(r)=-\frac{F^{\prime }(r)}{r}\left(1-\frac{b(r)}{r}\right)+\frac{F(r)}{2r^3}[b(r)-r{b}^{\prime }(r)],$$

$$R(r)=\frac{2b^{\prime }(r)}{r^2}.$$

$$d{s}^2=-e^{\nu (r)}d{t}^2+e^{\lambda (r)}d{r}^2+r^2(d{\theta }^2+{\text{sin}}^2\theta d{\varphi }^2).$$

$$8\pi \rho =e^{-\lambda }\left(\frac{{\lambda }^{\prime }}{r}-\frac{1}{r^2}\right)+\frac{1}{r^2},$$

$$8\pi p_r=e^{-\lambda }\left(\frac{1}{r^2}+\frac{{\nu }^{\prime }}{r}\right)-\frac{1}{r^2},$$

$$8\pi p_t=\frac{1}{2}{e}^{-\lambda }\left[\frac{1}{2}({\nu }^{\prime }{)}^2+{\nu }^{\prime \prime }-\frac{1}{2}{\lambda }^{\prime }{\nu }^{\prime }+\frac{1}{r}({\nu }^{\prime }-{\lambda }^{\prime })\right].$$

$$8\pi \rho (r)=F(r)\left[e^{-\lambda }\left(\frac{{\lambda }^{\prime }}{r}-\frac{1}{r^2}\right)+\frac{1}{r^2}\right],$$

$$8\pi p_r(r)=F(r)\left[e^{-\lambda }\frac{1}{r^2}-\frac{1}{r^2}\right]+\frac{F^{\prime }(r)}{2}{\lambda }^{\prime }{e}^{-\lambda }-F^{\prime \prime }(r)e^{-\lambda },$$

$$8\pi p_t(r)=-\frac{F^{\prime }(r)}{r}{e}^{-\lambda }-\frac{F(r)}{2r}{\lambda }^{\prime }{e}^{-\lambda }.$$

$$\begin{gathered} \omega F(r)\left[e^{-\lambda }\left(\frac{{\lambda }^{\prime }}{r}-\frac{1}{r^2}\right)+\frac{1}{r^2}\right] \\ =F(r)\left[\frac{e^{-\lambda }}{r^2}-\frac{1}{r^2}\right]+\frac{F^{\prime }(r)}{2}{\lambda }^{\prime }{e}^{-\lambda }-F^{\prime \prime }(r)e^{-\lambda }. \end{gathered}$$

$$F^{\prime \prime }(r)-\frac{1}{2}{F}^{\prime }(r){\lambda }^{\prime }+F(r)\left[\omega \frac{{\lambda }^{\prime }}{r}+(\omega +1)\frac{1}{r^2}(e^{\lambda }-1)\right]=0.$$

$$d{s}^2=-d{t}^2+a^2(t)\left[\frac{d{r}^2}{1-k{r}^2}+r^2(d{\theta }^2+{\text{sin}}^2\theta d{\varphi }^2)\right].$$

$$e^{\lambda }=a^2(t)\frac{1}{1-k{r}^2}$$

$$\lambda =\text{ln}{a}^2(t)+\text{ln}(1-k{r}^2{)}^{-1},$$

$${\lambda }^{\prime }=\frac{2kr}{1-k{r}^2},$$

$$F^{\prime \prime }(r)-\frac{kr}{1-k{r}^2}{F}^{\prime }-\frac{2k}{1-k{r}^2}F=0.$$

$$F(r)=c_1\text{cos}[\sqrt{2}\text{ln}(|k|r+\sqrt{k^2{r}^2-1})]+c_2\text{sin}[\sqrt{2}\text{ln}(|k|r+\sqrt{k^2{r}^2-1})],k\ne 0.$$

$$F(r)=c\text{sin}[\sqrt{2}\text{ln}(|k|r+\sqrt{k^2{r}^2-1}+\varphi ],$$

$$g(r)=\text{sin}[\sqrt{2}\text{ln}(|k|r+\sqrt{k^2{r}^2-1}]\sim \text{sin}(\text{ln}r)$$

$$ar+b\approx b,-1\le b\le 1.$$

$$F(r)=c\text{sin}[\sqrt{2}\text{ln}(|k|r+\sqrt{k^2{r}^2-1}],$$

$$\sqrt{2}\text{ln}(|k|r+\sqrt{k^2{r}^2-1})=n\pi$$

$$r=\frac{1}{|k|}\text{cosh}\frac{n\pi }{2}.$$

$$r_1=\frac{1}{|k|}\text{cosh}\frac{n\pi }{2}\text{and}{r}_2=\frac{1}{|k|}\text{cosh}\frac{(n+1)\pi }{2}.$$

Full text

Keywords

Cosmological Constant, $f(R)$ Gravity

1 Introduction

The discovery that our Universe is undergoing an accelerated expansion [1, 2] has led to a renewed interest in modified theories of gravity. One of the most important of these, $f(R)$ modified gravity, replaces the Ricci scalar $R$ in the Einstein-Hilbert action

[TABLE]

by a nonlinear function $f(R)$:

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(For a review, see Refs. [3, 4, 5].)

An alternative to the modified gravity model is the hypothesis that the acceleration is due to a negative pressure dark energy, implying that $\overset{..}{a}>0$ in the Friedmann equation

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(We are using units in which $c=G=1$.) In the equation of state $p=\omega\rho$, $\overset{..}{a}>0$ corresponds to the range of values $\omega<-1/3$, referred to as quintessence dark energy. The case $\omega=-1$ is equivalent to assuming Einstein’s cosmological constant. It has been forcefully argued by Bousso [6] that the cosmological constant is the best model for dark energy. In this note we go a step further and propose that $f(R)$ modified gravity implies that $\omega=-1$ is the only allowed value in the equation of state $p=\omega\rho$.

2 The solution

For convenience of notation, we start with the spherically symmetric line element

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It was shown by Lobo [7] that under the assumption that $\Phi^{\prime}(r)\equiv 0$, the Einstein field equations are

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and

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where $F=\frac{df}{dR}$. The curvature scalar $R$ is given by

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For our purposes, a more convenient form of the line element is

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Here the Einstein field equations can be written [8]

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and

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Then if $\nu^{\prime}\equiv 0$, Lobo’s equations become

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and

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Now substituting into the equation of state $p=\omega\rho$, we obtain

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This equation can be rewritten as follows:

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Since we are dealing with a cosmological setting, we may assume the FLRW model, so that $\nu\equiv 0$:

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Observe that we now have

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and

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so that

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which is independent of time. The significance of the special value $\omega=-1$ in Eq. (14) now becomes apparent: the entire equation has become time independent, i.e.,

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(For later reference, observe that if $k=0$, then $F(r)=c_{1}+c_{2}r$.) The solution of Eq. (19) is

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This solution can also be written

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where $c=\sqrt{c_{1}^{2}+c_{2}^{2}}$ and $\phi=\text{tan}^{-1}(c_{1}/c_{2})$.

3 Staying close to Einstein gravity

In a cosmological setting, $f(R)$ modified gravity must remain close to Einstein gravity to be consistent with observation. In this section we wish to show that it is possible, at least in principle, to choose the arbitrary constants in Eq. (21) so that this goal is achieved.

The sinusoidal solution (21) has a large period and a small slope, especially for large $r$. To confirm this statement, observe that the function

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for large $r$. So both $g^{\prime}(r)$ and $g^{\prime\prime}(r)$ approach zero as $r\rightarrow\infty$. As a result, $\text{sin}(\text{ln}\,r)$ has the approximate form $ar+b$ on any interval that is not excessively large, and since the slope $a$ is small in absolute value, we have

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We can now show that it is possible in principle to choose the arbitrary constants $c$ and $\phi$ in such a way that $F(r)$ remains close to unity and both $F^{\prime}$ and $F^{\prime\prime}$ close to zero on one complete period.

Let $\phi=0$, so that

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First observe that $F(r)=0$ whenever

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for all integers $n$. Solving for $r$, we get

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Now choose a particular $n$ for which $F(r)\geq 0$ on the interval $[r_{1},r_{2}]$, where

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Next, subdivide the interval $[r_{1},r_{2}]$ into $i$ subintervals $I_{i}$ each of which is small enough so that $b$ remains in a narrow range. Then on each separate subinterval, construct a tangent line $a_{i}r+b_{i}\approx b_{i}$ near the midpoint, thereby ensuring that $b_{i}\neq 0$. (See Fig. 1.) So we may now choose $c_{i}=1/b_{i}$

for the arbitrary constant $c$. We then repeat the procedure on the interval $[r_{2},r_{2}+\pi]$, so that $F(r)\approx 1$ on the entire period $[r_{1},r_{2}+\pi]$. Since both $F^{\prime}$ and $F^{\prime\prime}$ are close to zero [from Eq. (22)], the periodicity of $F(r)$ guarantees that our $f(R)$ modified gravity is close to Einstein gravity for all $r$.

4 The cosmological constant

Suppose we return to Eq. (14) and substitute Eqs. (16)-(18). Then we obtain

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While we normally assume that $k\neq 0$, it is noted in Ref. [3] that $k=0$, representing a spatially flat Universe, is not a dramatic departure from generality when it comes to late-time cosmology.

With $k=0$, the time-dependent solution is

[TABLE]

In the special case $\omega=-1$, $F(r)=c_{1}+c_{2}r$, in agreement with Eq. (19) with $k=0$.

In the previous section we dealt with a time-independent solution due to the assumption $\omega=-1$. This allowed our $f(R)$ modified model to remain close to Einstein gravity at least in principle. By contrast, solution (27) is time dependent. So if $\omega\neq-1$, we are dealing with two possibilities:

(a) if $\omega>-1$, there is no real solution;

(b) if $\omega<-1$, then the $f(R)$ model is far removed from Einstein gravity, i.e., if $a^{2}(t)$ increases indefinitely, then the first term in solution (27) goes to zero, while the second term gets large. So $F(r)$ cannot remain close to unity.

We conclude that $\omega=-1$ in the equation of state $p=\omega\rho$ is the only allowed value. Since this note deals with rather reasonable assumptions, the only plausible objection to this conclusion is that the equation of state for dark energy is much more complicated than the perfect-fluid equation of state $p=\omega\rho$. This possibility was also raised by Lobo [5], who stated that a mixture of various interacting non-ideal fluids may be necessary. This could imply that dark energy is dynamic in nature, thereby forcing us to exclude models with constant $\omega$, including the cosmological constant.

It should be noted that similar conclusions were reached in Ref. [9] using a different and somewhat more general approach.

5 Conclusion

The starting point in this note is $f(R)$ modified gravity in a cosmological setting. We also assume a spatially flat Universe to describe late-time cosmology [3]; thus $k=0$ in the FLRW model. Our key assumption is the perfect-fluid equation of state $p=\omega\rho$ to describe the hypothesized dark energy. While $\omega<-1/3$ is sufficient to yield an accelerated expansion, it was concluded that $\omega=-1$ is the only value that allows our solution to remain close enough to Einstein gravity to be consistent with observation.

Weighing the above assumptions, we conclude that either (1) Einstein’s cosmological constant is the only acceptable model for dark energy or (2) that the equation of state is far more complicated than the above perfect-fluid equation and may even exclude a constant $\omega$.