Hamiltonian constraint

In its usual presentation, classical mechanics appears to give time a special role as an independent variable. This is unnecessary, however. Mechanics can be formulated to treat the time variable on the same footing as the other variables in an extended phase space, by parameterizing the temporal variable(s) in terms of a common, albeit unspecified parameter variable. Phase space variables being on the same footing.

We introduce ${\displaystyle \tau }$ as an unphysical parameter labeling different possible correlations between the time reading ${\displaystyle t}$ of the clock and the elongation ${\displaystyle x}$ of the pendulum. ${\displaystyle \tau }$ is unphysical parameter and there are many different choices for it.

Say our system comprised a pendulum executing a simple harmonic motion and a clock. Whereas the system could be described classically by a position x=x(t), with x defined as a function of time, it is also possible to describe the same system as x(${\displaystyle \tau }$) and t(${\displaystyle \tau }$) where the relation between x and t is not directly specified. Instead, x and t are determined by the parameter ${\displaystyle \tau }$, which is simply a parameter of the system, possibly having no objective meaning in its own right.

The system would be described by the position of a pendulum from the center, denoted ${\displaystyle x}$, and the reading on the clock, denoted ${\displaystyle t}$. We put these variables on the same footing by introducing a fictitious parameter ${\displaystyle \tau }$,

${\displaystyle x(\tau ),\;\;\;\;t(\tau )}$

whose `evolution' with respect to ${\displaystyle \tau }$ takes us continuously through every possible correlation between the displacement and reading on the clock. Obviously the variable ${\displaystyle \tau }$ can be replaced by any monotonic function, ${\displaystyle \tau '=f(\tau )}$. This is what makes the system reparametrisation-invariant. Note that by this reparametrisation-invariance the theory cannot predict the value of ${\displaystyle x(\tau )}$ or ${\displaystyle t(\tau )}$ for a given value of ${\displaystyle \tau }$ but only the relationship between these quantities. Dynamics is then determined by this relationship.

The action for the parametrized Harmonic oscillator is then

${\displaystyle S=\int d\tau {\Big [}{dx \over d\tau }p+{dt \over d\tau }p_{t}-\lambda {\Big (}p_{t}+{p^{2} \over 2m}+{1 \over 2}m\omega ^{2}x^{2}{\Big )}{\Big ]}.}$

where ${\displaystyle x}$ and ${\displaystyle t}$ are canonical coordinates and ${\displaystyle p}$ and ${\displaystyle p_{t}}$ are their conjugate momenta respectively and represent our extended phase space (we will show that we can recover the usual Newton's equations from this expression). Writing the action as

${\displaystyle S=\int d\tau {\Big [}{dx \over d\tau }p+{dt \over d\tau }p_{t}-{\mathcal {H}}(x,t;p,p_{t}){\Big ]}}$

we identify the ${\displaystyle {\mathcal {H}}}$ as

${\displaystyle {\mathcal {H}}(x,t,\lambda ;p,p_{t})=\lambda {\Big (}p_{t}+{p^{2} \over 2m}+{1 \over 2}m\omega ^{2}x^{2}{\Big )}.}$

Hamilton's equations for ${\displaystyle \lambda }$ are

${\displaystyle {\partial {\mathcal {H}} \over \partial \lambda }=0}$

which gives a constraint,

${\displaystyle C=p_{t}+{p^{2} \over 2m}+{1 \over 2}m\omega ^{2}x^{2}=0.}$

${\displaystyle C}$ is our Hamiltonian constraint! It could also be obtained from the Euler–Lagrange equation of motion, noting that the action depends on ${\displaystyle \lambda }$ but not its ${\displaystyle \tau }$ derivative. Then the extended phase space variables ${\displaystyle x}$, ${\displaystyle t}$, ${\displaystyle p}$, and ${\displaystyle p_{t}}$ are constrained to take values on this constraint-hypersurface of the extended phase space. We refer to ${\displaystyle \lambda C}$ as the `smeared' Hamiltonian constraint where ${\displaystyle \lambda }$ is an arbitrary number. The `smeared' Hamiltonian constraint tells us how an extended phase space variable (or function thereof) evolves with respect to ${\displaystyle \tau }$:

${\displaystyle {dx \over d\tau }=\{x,\lambda C\},\;\;\;\;{dp \over d\tau }=\{p,\lambda C\}\;\;\;\;\;\;{dt \over d\tau }=\{t,\lambda C\},\;\;\;\;{dp_{t} \over d\tau }=\{p_{t},\lambda C\}}$

(these are actually the other Hamilton's equations). These equations describe a flow or orbit in phase space. In general we have

${\displaystyle {dF(x,p,t,p_{t}) \over d\tau }=\{F(x,p,t,p_{t}),\lambda C\}}$

for any phase space function ${\displaystyle F}$. As the Hamiltonian constraint Poisson commutes with itself, it preserves itself and hence the constraint-hypersurface. The possible correlations between measurable quantities like ${\displaystyle x(\tau )}$ and ${\displaystyle t(\tau )}$ then correspond to `orbits' generated by the constraint within the constraint surface, each particular orbit differentiated from each other by say also measuring the value of say ${\displaystyle p(\tau )}$ along with ${\displaystyle x(\tau )}$ and ${\displaystyle t(\tau )}$ at one ${\displaystyle \tau }$-instant; after determining the particular orbit, for each measurement of ${\displaystyle t(\tau )}$ we can predict the value ${\displaystyle x(\tau )}$ will take.

The other equations of Hamiltonian mechanics are

${\displaystyle {dx \over d\tau }={\partial {\mathcal {H}} \over \partial p},\;\;\;\;{dp \over d\tau }=-{\partial {\mathcal {H}} \over \partial x};\;\;\;\;\;\;{dt \over d\tau }={\partial {\mathcal {H}} \over \partial p_{t}},\;\;\;\;{dp_{t} \over d\tau }={\partial {\mathcal {H}} \over \partial t}.}$

Upon substitution of our action these give,

${\displaystyle {dx \over d\tau }=\lambda {p \over m},\;\;\;\;{dp \over d\tau }=-\lambda m\omega ^{2}x;\;\;\;\;\;\;{dt \over d\tau }=\lambda ,\;\;\;\;{dp_{t} \over d\tau }=0,}$

These represent the fundamental equations governing our system.

In the case of the parametrized clock and pendulum system we can of course recover the usual equations of motion in which ${\displaystyle t}$ is the independent variable:

Now ${\displaystyle dx/dt}$ and ${\displaystyle dp/dt}$ can be deduced by

${\displaystyle {dx \over dt}={dx \over d\tau }{\Big /}{dt \over d\tau }={\lambda p/m \over \lambda }={p \over m}}$

${\displaystyle {dp \over dt}={dp \over d\tau }{\Big /}{dt \over d\tau }={-\lambda m\omega ^{2}x \over \lambda }=-m\omega ^{2}x.}$

We recover the usual differential equation for the simple harmonic oscillator,

${\displaystyle {d^{2}x \over dt^{2}}=-\omega ^{2}x.}$

We also have ${\displaystyle dp_{t}/dt=dp_{t}/d\tau {\big /}dt/d\tau =0}$ or ${\displaystyle p_{t}=Const.}$

Our Hamiltonian constraint is then easily seen as the condition of constancy of energy! Deparametrization and the identification of a time variable with respect to which everything evolves is the opposite process of parametrization. It turns out in general that not all reparametrisation-invariant systems can be deparametrized. General relativity being a prime physical example (here the spacetime coordinates correspond to the unphysical ${\displaystyle \tau }$ and the Hamiltonian is a linear combination of constraints which generate spatial and time diffeomorphisms).

The underlining reason why we could deparametrize (aside from the fact that we already know it was an artificial reparametrization in the first place) is the mathematical form of the constraint, namely,

${\displaystyle C=p_{t}+C'(x,p)}$.

Substitute the Hamiltonian constraint into the original action we obtain

${\displaystyle S=\int d\tau {\Big [}{dx \over d\tau }p+{dt \over d\tau }p_{t}-\lambda (p_{t}+C'(x,p)){\Big ]}}$

${\displaystyle =\int d\tau {\Big [}{dx \over d\tau }p-{dt \over d\tau }C'(x,p){\Big ]}}$

${\displaystyle =\int dt{\Big [}{dx \over dt}p-{p^{2} \over 2m}+{1 \over 2}m\omega ^{2}x^{2}{\Big ]}}$

which is the standard action for the harmonic oscillator. General relativity is an example of a physical theory where the Hamiltonian constraint isn't of the above mathematical form in general, and so cannot be deparametrized in general.

The idea was to quantize the canonical variables ${\displaystyle q_{ab}}$ and ${\displaystyle \pi ^{ab}={\sqrt {q}}(K^{ab}-q^{ab}K_{c}^{c})}$, making them into operators acting on wavefunctions on the space of 3-metrics, and then to quantize the Hamiltonian (and other constraints). However, this program soon became regarded as dauntingly difficult for various reasons, one being the non-polynomial nature of the Hamiltonian constraint:

${\displaystyle H={\sqrt {det(q)}}(K_{ab}K^{ab}-(K_{a}^{a})^{2}-\;^{3}R)}$

where ${\displaystyle \;^{3}R}$ is the scalar curvature of the three metric ${\displaystyle q_{ab}(x)}$. Being a non-polynomial expression in the canonical variables and their derivatives it is very difficult to promote to a quantum operator.

The configuration variables of Ashtekar's variables behave like an ${\displaystyle SU(2)}$ gauge field or connection ${\displaystyle A_{a}^{i}}$. Its canonically conjugate momentum is ${\displaystyle {\tilde {E}}_{i}^{a}}$ is the densitized "electric" field or triad (densitized as ${\displaystyle {\tilde {E}}_{i}^{a}={\sqrt {det(q)}}E_{i}^{a}}$). What do these variables have to do with gravity? The densitized triads can be used to reconstruct the spatial metric via

${\displaystyle det(q)q^{ab}={\tilde {E}}_{i}^{a}{\tilde {E}}_{j}^{b}\delta ^{ij}}$.

The densitized triads are not unique, and in fact one can perform a local in space rotation with respect to the internal indices ${\displaystyle i}$. This is actually the origin of the ${\displaystyle SU(2)}$ gauge invariance. The connection can be used to reconstruct the extrinsic curvature. The relation is given by

${\displaystyle A_{a}^{i}=\Gamma _{a}^{i}-iK_{a}^{i}}$

where ${\displaystyle \Gamma _{a}^{i}}$ is related to the spin connection, ${\displaystyle \Gamma _{a\;\;i}^{\;\;j}}$, by ${\displaystyle \Gamma _{a}^{i}=\Gamma _{ajk}\epsilon ^{jki}}$ and ${\displaystyle K_{a}^{i}=K_{ab}{\tilde {E}}^{ai}/{\sqrt {det(q)}}}$.

In terms of Ashtekar variables the classical expression of the constraint is given by,

${\displaystyle H={\epsilon _{ijk}F_{ab}^{k}{\tilde {E}}_{i}^{a}{\tilde {E}}_{j}^{b} \over {\sqrt {det(q)}}}}$.

where ${\displaystyle F_{ab}^{k}}$ field strength tensor of the gauge field ${\displaystyle A_{a}^{i}}$ . Due to the factor ${\displaystyle 1/{\sqrt {det(q)}}}$ this is non-polynomial in the Ashtekar's variables. Since we impose the condition

${\displaystyle H=0}$,

we could consider the densitized Hamiltonian instead,

${\displaystyle {\tilde {H}}={\sqrt {det(q)}}H=\epsilon _{ijk}F_{ab}^{k}{\tilde {E}}_{i}^{a}{\tilde {E}}_{j}^{b}=0}$.

This Hamiltonian is now polynomial the Ashtekar's variables. This development raised new hopes for the canonical quantum gravity programme.[5] Although Ashtekar variables had the virtue of simplifying the Hamiltonian, it has the problem that the variables become complex. When one quantizes the theory it is a difficult task ensure that one recovers real general relativity as opposed to complex general relativity. Also there were also serious difficulties promoting the densitized Hamiltonian to a quantum operator.

A way of addressing the problem of reality conditions was noting that if we took the signature to be ${\displaystyle (+,+,+,+)}$, that is Euclidean instead of Lorentzian, then one can retain the simple form of the Hamiltonian for but for real variables. One can then define what is called a generalized Wick rotation to recover the Lorentzian theory.[6] Generalized as it is a Wick transformation in phase space and has nothing to do with analytical continuation of the time parameter ${\displaystyle t}$.

Thomas Thiemann addressed both the above problems.[4] He used the real connection

${\displaystyle A_{a}^{i}=\Gamma _{a}^{i}+\beta K_{a}^{i}}$

In real Ashtekar variables the full Hamiltonian is

${\displaystyle H=-\zeta {\epsilon _{ijk}F_{ab}^{k}{\tilde {E}}_{i}^{a}{\tilde {E}}_{j}^{b} \over {\sqrt {det(q)}}}+2{\zeta \beta ^{2}-1 \over \beta ^{2}}{({\tilde {E}}_{i}^{a}{\tilde {E}}_{j}^{b}-{\tilde {E}}_{j}^{a}{\tilde {E}}_{i}^{b}) \over {\sqrt {det(q)}}}(A_{a}^{i}-\Gamma _{a}^{i})(A_{b}^{j}-\Gamma _{b}^{j})=H_{E}+H'}$.

where the constant ${\displaystyle \beta }$ is the Barbero-Immirzi parameter.[7] The constant ${\displaystyle \zeta }$ is -1 for Lorentzian signature and +1 for Euclidean signature. The ${\displaystyle \Gamma _{a}^{i}}$ have a complicated relationship with the densitized triads and causes serious problems upon quantization. Ashtekar variables can be seen as choosing ${\displaystyle \beta =i}$ to make the second more complicated term was made to vanish (the first term is denoted ${\displaystyle H_{E}}$ because for the Euclidean theory this term remains for the real choice of ${\displaystyle \beta =\pm 1}$). Also we still have the problem of the ${\displaystyle 1/{\sqrt {det(q)}}}$ factor.

Thiemann was able to make it work for real ${\displaystyle \beta }$. First he could simplify the troublesome ${\displaystyle 1/{\sqrt {det(q)}}}$ by using the identity

${\displaystyle \{A_{c}^{k},V\}={\epsilon _{abc}\epsilon ^{ijk}{\tilde {E}}_{i}^{a}{\tilde {E}}_{j}^{b} \over {\sqrt {det(q)}}}}$

where ${\displaystyle V}$ is the volume,

${\displaystyle V=\int d^{3}x{\sqrt {det(q)}}={1 \over 6}\int d^{3}x{\sqrt {|{\tilde {E}}_{i}^{a}{\tilde {E}}_{j}^{b}{\tilde {E}}_{k}^{c}\epsilon ^{ijk}\epsilon _{abc}|}}}$.

The first term of the Hamiltonian constraint becomes

${\displaystyle H_{E}=\{A_{c}^{k},V\}F_{ab}^{k}{\tilde {\epsilon }}^{abc}}$

upon using Thiemann's identity. This Poisson bracket is replaced by a commutator upon quantization. It turns out that a similar trick can be used to teat the second term. Why are the ${\displaystyle \Gamma _{a}^{i}}$ given by the densitized triads ${\displaystyle {\tilde {E}}_{i}^{a}}$? It actually come about from the Gauss Law

${\displaystyle D_{a}{\tilde {E}}_{i}^{a}=0}$.

We can solve this in much the same way as the Levi-Civita connection can be calculated from the equation ${\displaystyle \nabla _{c}g_{ab}=0}$; by rotating the various indices and then adding and subtracting them. The result is complicated and non-linear. To circumvent the problems introduced by this complicated relationship Thiemann first defines the Gauss gauge invariant quantity

${\displaystyle K=\int d^{3}xK_{a}^{i}{\tilde {E}}_{i}^{a}}$

where ${\displaystyle K_{a}^{i}=K_{ab}{\tilde {E}}^{ai}/{\sqrt {det(q)}}}$, and notes that

${\displaystyle K_{a}^{i}=\{A_{a}^{i},K\}}$.

We are then able to write

${\displaystyle A_{a}^{i}-\Gamma _{a}^{i}=\beta K_{a}^{i}=\beta \{A_{a}^{i},K\}}$

and as such find an expression in terms of the configuration variable ${\displaystyle A_{a}^{i}}$ and ${\displaystyle K}$. We obtain for the second term of the Hamiltonian

${\displaystyle H'=\epsilon ^{abc}\epsilon _{ijk}\{A_{a}^{i},K\}\{A_{b}^{j},K\}\{A_{c}^{k},V\}}$.

Why is it easier to quantize ${\displaystyle K}$? This is because it can be rewritten in terms of quantities that we already know how to quantize. Specifically ${\displaystyle K}$ can be rewritten as

${\displaystyle K=-\{V,\int d^{3}xH_{E}\}}$

where we have used that the integrated densitized trace of the extrinsic curvature is the "time derivative of the volume".