A nearly complete fragment of a paper on Loop Quantum Cosmology identifying a simple form of Hamiltonian constraint operator for Bianchi I.

It is possible that these results were incorporated into published research.

A Simple Form of the Bianchi I ConstraintPermalink

IntroductionPermalink

Loop Quantum Cosmology - the application of the principles of Loop Quantum Gravity to symmetry reduced cosmological models - has quickly developed into an active field of research. The homogeneous and isotropic FLRW model has been intensely analyzed. The k=0 model is exactly soluble - allowing one to analytically observe that the big bang is transformed by quantum effects into a big ‘bounce’ and determine an upper bound on the energy density. Extensive numerical evolutions have been run for these models showing how semiclassical states evolve through the bounce.
For the anisotropic models though the complexity of the constraint operator has limited analysis to the effective semi-classical equations of motion. While the Hamiltonian constraint operator for FLRW and Binachi I both preserve a regular lattice in the volume, the Bianchi I constraint takes values on a dense subset of the reals in the anisotropic parameters. This poses complications for any numerical analysis - looking for eigenstates of the constraint, with numerical evolution of semi-classical states,…

In this paper we present a dramatic simplification of the Bianchi I constraint allowing for both numerical evolution and possibly analytical study. I will overview the classical framework then the loop quantum quantization and finally the simplification. Given the simplification I will probe the spectrum of the constraint operator.

Classical FrameworkPermalink

We introduce a fiducial metric ${}^o q_{ab}$, ${}^o ds^2 = dx^2+dy^2+dz^2$, and a fiducial cell $V$ whose edges lie along the coordinates directions $x,y,z$. The fiducial cell has edge lengths $L_i$ and volume ${}^oV=L_1L_2L_3$ as measured by the fiducial metric.

Due the symmetries of the model the connection and triad can be reduced to the following form

$$\begin{equation} A_a^i =: c^i (L^i)^{-1} {}^o \omega_a^i \quad E^a_i =: p_i L_i V_o^{-1} \sqrt{^o q} {}^o e^a_i \end{equation}$$

Where the connection is determined entirely by the three variables $c_i$ and the triad by the three variables $p_i$. They have the following simple Poisson bracket.

$$\begin{equation} { c^i,p_j } = 8\pi G \delta^i_j \end{equation}$$

In this form the connection and triad automatically solve the Gauss and diffeomorphism constraints leaving only the scalar constraint. The choice of harmonic time, catered to the use of the scalar field as a clock, $N= \sqrt{\vert p_1 p_2 p_3 \vert}$ leads to the following form of the constraint

$$\begin{equation} \mathcal{C}_H = -\frac{1}{8\pi G \gamma^2} (p_1p_2c_1c_2+p_1p_3c_1c_3+p_2p_3c_2c_3) + \frac{p_T^2}{2} \end{equation}$$

Here the constraint is for Bianchi I with a massless the scalar field, but in this paper we will focus mostly on the gravitational part of the constraint. From the constraint we find that we there are three constants of motion $c_i p_i$ (no summation), which commute trivially with the constraint.

The relation of $c,p$ to the scale factor is given by

$$\begin{align} p_1 &= sgn(a_1) |a_2 a_3| L_2 L_3 \newline\nonumber p_2 &= sgn(a_2) |a_1 a_3| L_1 L_3 \newline\nonumber p_3 &= sgn(a_3) |a_1 a_2| L_1 L_2 \end{align}$$

and

$$\begin{equation} c_i= \gamma L_i V_o^{-1} (a_1a_2a_3)^{-1} \frac{d a_i}{d\tau} \end{equation}$$

where the equations of motion are used to show that the c’s are related to the time derivative of the scale factor. The constants of motion are then

$$\begin{equation} p_i c_i = \gamma \frac{1}{a} \frac{d a_i}{d \tau}, \end{equation}$$

which are related to the expansion rate along each direction. These constants will be relevant to the interpretation of the simplification of the quantum constraint.

Quantum KinematicsPermalink

As in Loop Quantum Gravity we take the elementary variables to be the fluxes and holonomies. The fluxes are determined by the triad $p_i$. The holonomy along one of the coordinate directions is given by

$$\begin{equation} \label{hol} h_1^{(\ell)} (c_1,c_2,c_3) = \cos \frac{c_1\ell}{2} \mathbb{I} + 2 \sin \frac{c_1 \ell}{2} \tau_1 \end{equation}$$

which is an almost period function in c. Hence as our basic phase space variables we take $\exp (i\ell c_j)$ and $p_i$.

$$\begin{equation} { e^{i \ell c_j},p_i } = i \ell e^{i \ell c_j} \delta_{ij} \end{equation}$$

In the holonomy representation the Hilbert space consists of wave functions $\Psi(c)$ with finite norm

$$\begin{equation} || \Psi ||^2 = \underset{\alpha \rightarrow \infty}{lim} \frac{1}{2\alpha} \int_{-\alpha}^{\alpha} \textrm{d} c |\Psi(c)|^2 \end{equation}$$

Where holonomies act by multiplication and $p_i$ acts by differentiation.

$$\begin{equation} \hat{e^{i \ell c}} \Psi(c) = e^{i \ell c} \Psi(c) \quad \hat{p_i} \Psi(c) = -i \partial_c \Psi(c) \end{equation}$$

The space is the space of square integrable function on the Bohr compactification of $\mathbb{R}$. The non-existence of the operator c can be seen clearly since normalizable states are those that are asymptotically constant. Any state that has non-zero finite norm will be mapped to a state with infinite norm by the action of $c$.

On the other hand we can work in the conjugate representation where the Hilbert space consists of wave function $\Psi(p)$ with finite norm

$$\begin{equation} || \Psi ||^2 = \sum_p | \Psi(p)|^2 \end{equation}$$

where the sum here is over all real numbers. In the representation the $p$’s act by multiplication and the holonomies by translations.

$$\begin{equation} \hat{p} \Psi(p) = p \Psi(p) \quad \hat{e^{i \ell c}} \Psi(p) = \Psi(c + \ell) \end{equation}$$

The ‘fourier transform’ between these two representations is given by

$$\begin{equation} \tilde{\Psi}(p) = \underset{\alpha \rightarrow \infty}{lim} \frac{1}{2\alpha} \int_{-\alpha}^{\alpha} \textrm{d} c \,e^{i c p} \Psi(c) \end{equation}$$

with the inverse given by

$$\begin{equation} \Psi(c) = \sum_p e^{-i c p} \tilde{\Psi}(p) \end{equation}$$

For simplicity the dynamics are presented in the triad representation, but the simplification of the constraint is present in the holonomy representation.

ConstraintPermalink

To obtain the dynamics of the theory we need to represent the constraint as an operator on our kinematical hilbert space. This requires writing our constraint

$$\begin{equation} \mathcal{H} = \frac{E^a_i E^b_j}{16\pi G\sqrt{\vert q \vert}}\left( \epsilon^{ijk} F^k_{ab} -2(1+\gamma^2)K_{[a}^i K_{b]}^j \right) \end{equation}$$

in terms of the basic variables, which requires writing the curvature in terms of the holonomies around square loops along the coordinate directions.

$$\begin{equation} \label{F1} F_{ab}{}^k = 2\lim_{Ar_\Box\rightarrow 0}\,\, \mathrm{Tr}\left(\frac{h_{\Box_{ij}}- \mathbb{I}} {Ar_\Box} \tau^k\right)\,{}^o\omega_a^i{}^o\omega_b^j, \end{equation}$$

From the non-existence of an operator corresponding to the connection the limit $Ar_\Box\rightarrow 0$ does not exist. If we chose the physical area of the loop to be the smallest area eigenvalue of loop quantum gravity, the lengths of the holonomies are fixed to be

and the constraint is written in terms of operators

$$\begin{equation} \exp^{i c_i \bar\mu_i} \end{equation}$$

which have very complex action on the states $\Psi(p_1,p_2,p_3)$.

Much like in the FLRW models the action of these holonomies is simplified if we change variables to $\lambda_i$ defined by,

$$\begin{equation} \lambda_i\, =\, \frac{\rm{sgn}(p_i)\,\sqrt{|p_i|}}{(4\pi |\gamma|\, \sqrt\Delta\, {\ell}_{\rm Pl}^3)^{1/3}}\, , \end{equation}$$

and the action of the constraint is further simplified is we introduce the volume

$$\begin{equation} v = 2\lambda_1 \lambda_2 \lambda_3 \end{equation}$$

under these change of variables our Hilbert space is now functions of $\lambda_1,\lambda_2$, and $v$, all restricted to be positive, with finite norm.

$$\begin{equation} || \Psi ||^2 = \sum_{\lambda_1, \lambda_2, v} |\Psi(\lambda_1,\lambda_2,v)|^2 < \infty \end{equation}$$

The action of the constraint on wave functions of $\lambda_1,\lambda_2$, and $v$ takes the following simplified form.

$$\begin{align} \Theta \Psi(\lambda_1,\lambda_2,v) = \frac{\pi G}{2} \sqrt{v} &\left[-(v+2) \sqrt{v+4} \Psi_4^+(\lambda_1,\lambda_2,v) \right. \newline\nonumber & +(v+2) \sqrt{v} \Psi_0^+ (\lambda_1,\lambda_2,v) \newline\nonumber & +(v-2) \sqrt{v} \Psi_0^- (\lambda_1,\lambda_2,v) \newline \nonumber & \left.- (v-2) \sqrt{v-4} \Psi_4^-(\lambda_1,\lambda_2,v) \right] \end{align}$$

Which surprisingly acts as a difference operator in the volume v much like the FLRW models. There is one term that shifts the volume forward by 4, two that leave the volume the same, and one that shifts the volume back by 4. The complexity of the action of the constraint arises in how it changes the anistropies labelled by $\lambda_i$. The action on the anisotropies is given by multiplicative shifts depending on the volume.

$$\begin{align} \Psi^\pm_4(\lambda_1,\lambda_2,v)=\,& \Psi\left(\frac{v\pm4}{v\pm2}\lambda_1,\frac{v\pm2}{v}\lambda_2, v\pm4\right)+\Psi\left(\frac{v\pm4}{v\pm2}\lambda_1,\lambda_2, v\pm4\right)\nonumber\newline & +\Psi\left(\frac{v\pm2}{v}\lambda_1, \frac{v\pm4}{v\pm2}\lambda_2,v\pm4\right)+\Psi \left(\frac{v\pm2}{v}\lambda_1, \lambda_2,v\pm4\right)\nonumber \newline &+\Psi\left(\lambda_1,\frac{v\pm2}{v}\lambda_2, v\pm4\right)+\Psi\left(\lambda_1,\frac{v\pm4}{v\pm2}\lambda_2,v\pm4\right) \end{align}$$

$$\begin{align} \label{qham8} \Psi^\pm_0(\lambda_1,\lambda_2,v)=\, & \Psi\left(\frac{v\pm2}{v}\lambda_1, \frac{v}{v\pm2}\lambda_2,v\right) +\Psi\left(\frac{v\pm2}{v}\lambda_1,\lambda_2,v \right)\nonumber \newline &+\Psi\left(\frac{v}{v\pm2}\lambda_1,\frac{v\pm2}{v}\lambda_2,v \right)+\Psi\left(\frac{v}{v\pm2}\lambda_1,\lambda_2,v\right)\nonumber \newline & +\Psi\left(\lambda_1,\frac{v}{v\pm2}\lambda_2,v\right)+\Psi\left(\lambda_1,\frac{v\pm2}{v} \lambda_2,v\right) \end{align}$$

Where the action on the volume picks out nice invariant lattices. It can be seen that the invariant lattices in the anisotropies are isomorphic to the rationals and are thus dense in the space of all reals. It is here that the difficulty in analytical and numerical evaluation arise.

Simplification of ConstraintPermalink

Now we introduce a further simplification of the constraint. The first step is to introduce the simple change of variables $x_i = \ln(\lambda_i$. Under this change multiplicative shifts in $\lambda_i$ become translations in $x_i$. The range of variables goes from $\lambda$ ranging from $(0,\infty)$ to $x$ ranging from $(-\infty,\infty)$. And the measure changes simply since the change of variables in one to one $\sum_\lambda = \sum_x$. Further it is simple to see that the constraint commutes with all translations in $x$. We can then simultaneously diagonalize the constraint operator and the operators’ generating translations.

$$\begin{align} U_1(a) \Psi(\lambda_1,\lambda_2,v) = \Psi(\lambda_1+a,\lambda_2,v) \newline \left[ \Theta, U_i(a) \right] = 0 \end{align}$$

The eigenstates of translations are exponentials as we expect, $e^{i x_i m_i}$. We can then go to the dual representation, $\Psi(m_i,m_2, v)$.

$$\begin{equation} \Psi(m_1,m_2,v) = \sum_{x_1,x_2} e^{-i m_1 x_1} e^{-i m_2 x_2} \Psi(x_1,x_2,v) \end{equation}$$

Surprisingly in this representation the constraint takes a very simple form, namely it reduces to a difference equation much like in the FRW models. The action of the constraint is given by

$$\begin{align} \Theta \Psi(m_1,m_2, v) = &-f_+^4(m_1,m_2,v) \Psi(m_1,m_2,v+4) \newline\nonumber &+ (f_+^0+f_-^0) \Psi(m_1,m_2,v)\newline\nonumber & - f_-^4(m_1,m_2,v) \Psi(m_1,m_2,v-4) \end{align}$$

The $m$ labels are unchanged by the action of $\Theta$ as we expect. The operator simply shifts the volume in steps of 4 as with the FLRW $\Theta$. The difference lies simply in the functions that multiply the shifts in volume. These functions are given by,

$$\begin{equation} f_\pm^4 = \frac{\pi G}{2} \sqrt{v} (v \pm 2) \sqrt{v \pm 4} \left( e^{i m_1 \ln(\frac{v\pm 4} {v\pm2})} e^{i m_2 \ln(\frac{v\pm2}{v})} +e^{i m_1 \ln(\frac{v\pm 4}{v\pm2})} + e^{i m_1 \ln(\frac{v\pm2}{v})} + m_1 \leftrightarrow m_2\right) \end{equation}$$

and

$$\begin{equation} f_\pm^0 = \frac{\pi G}{2} \sqrt{v} (v \pm 2) \sqrt{v} \left( e^{i m_1 \ln(\frac{v} {v\pm2})} e^{i m_2 \ln(\frac{v\pm2}{v})} +e^{i m_1 \ln(\frac{v} {v\pm2})} + e^{i m_1 \ln(\frac{v\pm2}{v})} + m_1 \leftrightarrow m_2\right) \end{equation}$$

While these functions are complicated, for fixed values of $m_i$ it is a standard difference equation, which can be analyzed using standard tools.

InterpretationPermalink

We have seen that by carrying out a fourier transform to the variables conjugate to $x_i$ the constraint simplifies dramatically, but what has happened physically? What is the classical variable associated to the $m_i$? Classically we find that the canonically pair is given by

$$\begin{align} x_i = \ln \left( \frac{\sqrt{|p_i|}}{(4\pi |\gamma|\, \sqrt\Delta\, {\ell}_{\rm Pl}^3)^{1/3}} \right) \newline m_1 = 2(p_1 c_1 - p_3 c_3) \quad m_2 = 2(p_2 c_2 - p_3 c_3) \end{align}$$

We see that these commute with the volume

$$\begin{equation} {m_i, v } =0 \end{equation}$$

The conjugate to the volume is given by

$$\begin{equation} b = \frac{2}{3 v} (p_1 c_1 + p_2 c_2 + p_3 c_3) \end{equation}$$

So we can similarly that the $m_i$ commute with the conjugate to the volume. We then have a canonical transformation from $(c_i,p_i)$ to $(x_i,m_i,v,b)$. Recall that classically $p_i c_i$ was related to the hubble rate in the i-th direction. The $m_i$ then define the difference in the Hubble rates between the 3 direction - or describe the anisotropy of the system.

We then see that taking $m_i=0$ is equivalent to enforcing isotropy, and indeed if $m_i=0$ the constraint reduces to that of the $k=0$ FRLW model. How does this projection compare with that done in \cite{aew}. The original projection introduced was,

$$\begin{equation} \Psi_{FRW} = \sum_{\lambda_1,\lambda_2} \Psi(\lambda_1,\lambda_2,v) \end{equation}$$

Translating this to the variables $x_i$ and then taking the fourier transform we find that

$$\begin{equation} \Psi_{FRW} = \sum_{x_1,x_2} \underset{\alpha \rightarrow \infty}{lim} \frac{1}{2\alpha_1} \int_{-\alpha_1}^{\alpha_1} \textrm{d} m_1 \underset{\alpha \rightarrow \infty}{lim} \frac{1}{2\alpha_2} \int_{-\alpha_2}^{\alpha_2} \textrm{d} m_2 e^{i m_1 x_1} e^{i m_2 x_2} \Psi(m_1,m_2,v) \end{equation}$$

which reduces to

Where $\bar\delta(m)$ is the generalization of the Dirac delta distribution for the Bohr compactification, defined here in terms of its Fourier transform.

$$\begin{equation} \bar\delta(m) = \sum_{x} e^{i x m} \end{equation}$$

SpectrumPermalink

We can make a quick analysis of the spectrum of the operator to gain insight into the model. We know that in the FLRW k=0 model the Theta operator has a continuous spectrum $(0,\infty)$ and has $0$ as a discrete eigenvalue. The discrete eigenvalue given by the state with support on only the zero volume. This is reasonable since there are non-trivial solutions to the classical equations of motion without matter. On the other hand there are non-trivial solutions for vacuum Bianchi I, so how does the spectrum change. We would expect to see that the spectrum changes to include a non-trivial zero eigenvalue.

We can carry out an asymptotic expansion of the difference equation for large v, since the nature of the spectrum depends only on the asymptotic behavior - i.e. the normalizability of the eigenstates.

For large v the eigenvalue equation can be expanded as,

where now the functions have simplified to

$$\begin{equation} f_{\pm}^4 \rightarrow = 6v^2 \pm 8v \left(3+i(m_1+m_2) \right)+4\left(3+4i(m_1+m_2)-(m_1^2+m_2^2+(m_1+m_2)^2)\right) \end{equation}$$

$$\begin{equation} (f_+^0+f_-^0) = 12 v^2 - 8(m_1^2+m_2^2+(m_1-m_2)^2) \end{equation}$$

We can rearrange this equation by writing

If I can prove that the resulting left side is positive definite then we’re done, but I don’t think that it true.

Now we have an operator whose diagonal term is postiive, so it is more natural to assume that the constraint is positive definite. If it were we should see that the spectrum is continuous and runs from $(-m_1^2+m_2^2+(m_1-m_2)^2)$ to $\infty$.

In this case if we insert

$$\begin{equation} f_{\pm 4} = \frac{\pi G}{2} \sqrt{v} (v \pm 2) \sqrt{v \pm 4} \left[ 6 \pm \frac{8 i (m_1+m_2)}{v} - \frac{16 i (p_1+p_2)}{v^2} - \frac{8}{v^2} (m_1^2 + m_1 m_2 + m_2^2) \right] \end{equation}$$

$$\begin{equation} f_{\pm 0} = \frac{\pi G}{2} v (v \pm 2) \left[ 6 - \frac{8}{v^2} (m_1^2 - m_1 m_2 + m_2^2) \right] \end{equation}$$

We can numerically evolve the eigenvalue equation and look for the asymptotic behavior. When the state is normalizable with the kinematic inner product we have a state with a discrete spectrum. When the state is oscillatory and not divergent the value is part of the continuous spectrum, and when the state diverges there is no solution corresponding to that eigenvalue.

For the data obtained the eigenvalues $e$ are related to the original eigenvalues by

$$\begin{equation} \omega = 8\pi G\, e \end{equation}$$

As expected the $\Theta$ operator has a continuous spectrum that extends into the negative numbers. Further as the parameters labelling the anisotropy are increased the minimum eigenvalue becomes more and more negative and approaches $0$ as the parameters go to zero. From the numerical analysis we determine an approximate form for the minimum value to be $-\frac{16 \pi G}{3} (m_1^2+m_2^2+(m_1-m_2)^2)$.