Canonical transformation

Boldface variables such as represent a list of generalized coordinates that need not transform like a vector under rotation and similarly represents the corresponding generalized momentum, e.g., \begin{align} \mathbf{q} &\equiv \left (q_{1}, q_{2}, \ldots, q_{N-1}, q_{N} \right )\\ \mathbf{p} &\equiv \left (p_{1}, p_{2}, \ldots, p_{N-1}, p_{N} \right ). \end{align} A dot over a variable or list signifies the time derivative, e.g., \dot{\mathbf{q}} \equiv \frac{d\mathbf{q}}{dt}and the equalities are read to be satisfied for all coordinates, for example: \dot{\mathbf{p}} = -\frac{\partial f}{\partial \mathbf{q}}\quad \Longleftrightarrow \quad \dot = -\frac{\partial f}{\partial {q_i}} \quad (i = 1,\dots,N). The dot product notation between two lists of the same number of coordinates is a shorthand for the sum of the products of corresponding components, e.g., \mathbf{p} \cdot \mathbf{q} \equiv \sum_{k=1}^{N} p_{k} q_{k}. The dot product (also known as an "inner product") maps the two coordinate lists into one variable representing a single numerical value. The coordinates after transformation are similarly labelled with for transformed generalized coordinates and for transformed generalized momentum. == Conditions for restricted canonical transformation ==

Restricted canonical transformations are coordinate transformations where transformed coordinates and do not have explicit time dependence, i.e., \mathbf Q=\mathbf Q(\mathbf q,\mathbf p) and \mathbf P=\mathbf P(\mathbf q,\mathbf p) . The functional form of Hamilton's equations is \begin{align} \dot{\mathbf{p}} &= -\frac{\partial H}{\partial \mathbf{q}} \,, & \dot{\mathbf{q}} &= \frac{\partial H}{\partial \mathbf{p}} \end{align} In general, a transformation does not preserve the form of Hamilton's equations but in the case of a time independent transformation some simplifications are possible. Following the formal definition for a canonical transformation, it can be shown that for this type of transformation, the new Hamiltonian (sometimes called the Kamiltonian) can be expressed as: K(\mathbf Q, \mathbf P, t)= H(q(\mathbf Q,\mathbf P),p(\mathbf Q,\mathbf P),t) + \frac{\partial G}{\partial t}(t) where it differs from the Hamiltonian by a partial time derivative of a function known as a generator, which reduces to being only a function of time for restricted canonical transformations. In addition to leaving the form of the Hamiltonian unchanged, the Kamiltonian also permits the use of the unchanged Hamiltonian in Hamilton's equations of motion due to the above form as: \begin{alignat}{3} \dot{\mathbf{P}} &= -\frac{\partial K}{\partial \mathbf{Q}} &&= -\left(\frac{\partial H}{\partial \mathbf{Q}}\right)_{\mathbf Q,\mathbf P,t}\\ \dot{\mathbf{Q}} &= \,\,\,\, \frac{\partial K}{\partial \mathbf{P}} &&= \,\,\,\, \, \left(\frac{\partial H}{\partial \mathbf{P}}\right)_{\mathbf Q,\mathbf P ,t}\\ \end{alignat} Although the class of canonical transformations is larger than that which can be obtained with this restricted formulation, the restricted version provides a good starting point to obtain results that can be further generalized. All of the following conditions, with the exception of bilinear invariance condition, can be generalized for the full class of canonical transformations, including time dependence. Indirect conditions Since restricted transformations have no explicit time dependence (by definition), the time derivative of a new generalized coordinate is \begin{align} \dot{Q}_{m} &= \frac{\partial Q_{m}}{\partial \mathbf{q}} \cdot \dot{\mathbf{q}} + \frac{\partial Q_{m}}{\partial \mathbf{p}} \cdot \dot{\mathbf{p}} \\ &= \frac{\partial Q_{m}}{\partial \mathbf{q}} \cdot \frac{\partial H}{\partial \mathbf{p}} - \frac{\partial Q_{m}}{\partial \mathbf{p}} \cdot \frac{\partial H}{\partial \mathbf{q}} \\ &= \lbrace Q_m , H \rbrace \end{align} where {{math|{⋅, ⋅} }} is the Poisson bracket. Similarly for the identity for the conjugate momentum, Pm using the form of the "Kamiltonian" it follows that: \begin{align} \frac{\partial K(\mathbf{Q}, \mathbf{P}, t)}{\partial P_{m}} &= \frac{\partial K(\mathbf{Q}(\mathbf{q}, \mathbf{p}), \mathbf{P}(\mathbf{q}, \mathbf{p}), t)}{\partial \mathbf{q}} \cdot \frac{\partial \mathbf{q}}{\partial P_{m}} + \frac{\partial K(\mathbf{Q}(\mathbf{q}, \mathbf{p}), \mathbf{P}(\mathbf{q}, \mathbf{p}), t)}{\partial \mathbf{p}} \cdot \frac{\partial \mathbf{p}}{\partial P_{m}} \\[1ex] &= \frac{\partial H(\mathbf{q}, \mathbf{p}, t)}{\partial \mathbf{q}} \cdot \frac{\partial \mathbf{q}}{\partial P_{m}} + \frac{\partial H(\mathbf{q}, \mathbf{p}, t)}{\partial \mathbf{p}} \cdot \frac{\partial \mathbf{p}}{\partial P_{m}} \\[1ex] &= \frac{\partial H}{\partial \mathbf{q}} \cdot \frac{\partial \mathbf{q}}{\partial P_{m}} + \frac{\partial H}{\partial \mathbf{p}} \cdot \frac{\partial \mathbf{p}}{\partial P_{m}} \end{align} Due to the form of the Hamiltonian equations of motion, \begin{align} \dot{\mathbf{P}} &= -\frac{\partial K}{\partial \mathbf{Q}}\\ \dot{\mathbf{Q}} &= \,\,\,\, \frac{\partial K}{\partial \mathbf{P}} \end{align} if the transformation is canonical, the two derived results must be equal, resulting in the equations: \begin{align} \left( \frac{\partial Q_{m}}{\partial p_{n}}\right)_{\mathbf{q}, \mathbf{p}} &= -\left( \frac{\partial q_{n}}{\partial P_{m}}\right)_{\mathbf{Q}, \mathbf{P}} \\ \left( \frac{\partial Q_{m}}{\partial q_{n}}\right)_{\mathbf{q}, \mathbf{p}} &= \left( \frac{\partial p_{n}}{\partial P_{m}}\right)_{\mathbf{Q}, \mathbf{P}} \end{align} The analogous argument for the generalized momenta Pm leads to two other sets of equations: \begin{align} \left( \frac{\partial P_{m}}{\partial p_{n}}\right)_{\mathbf{q}, \mathbf{p}} &= \left( \frac{\partial q_{n}}{\partial Q_{m}}\right)_{\mathbf{Q}, \mathbf{P}} \\ \left( \frac{\partial P_{m}}{\partial q_{n}}\right)_{\mathbf{q}, \mathbf{p}} &= -\left( \frac{\partial p_{n}}{\partial Q_{m}}\right)_{\mathbf{Q}, \mathbf{P}} \end{align} These are the indirect conditions to check whether a given transformation is canonical. Symplectic condition Sometimes the Hamiltonian relations are represented as: \dot{\eta}= J \nabla_\eta H Where J := \begin{pmatrix} 0 & I_n \\ -I_n & 0 \\ \end{pmatrix}, and \mathbf{\eta} = \begin{bmatrix} q_1\\ \vdots \\ q_n\\ p_1\\ \vdots\\ p_n\\ \end{bmatrix} . Similarly, let \mathbf{\varepsilon} = \begin{bmatrix} Q_1\\ \vdots \\ Q_n\\ P_1\\ \vdots\\ P_n\\ \end{bmatrix} . From the relation of partial derivatives, converting the \dot{\eta}= J \nabla_\eta H relation in terms of partial derivatives with new variables gives \dot{\eta}=J ( M^T \nabla_\varepsilon H) where M := \frac{\partial (\mathbf{Q}, \mathbf{P})}{\partial (\mathbf{q}, \mathbf{p})}. Similarly for \dot{\varepsilon} , \dot{\varepsilon}=M\dot{\eta} =M J M^T \nabla_\varepsilon H Due to form of the Hamiltonian equations for \dot{\varepsilon} , \dot{\varepsilon}=J \nabla_\varepsilon K = J \nabla_\varepsilon H where \nabla_\varepsilon K = \nabla_\varepsilon H can be used due to the form of Kamiltonian. Equating the two equations gives the symplectic condition as: M J M^T = J The left hand side of the above is called the Poisson matrix of \varepsilon , denoted as \mathcal P(\varepsilon) = MJM^T . Similarly, a Lagrange matrix of \eta can be constructed as \mathcal L(\eta) = M^TJM . It can be shown that the symplectic condition is also equivalent to M^T J M = J by using the J^{-1}=-J property. The set of all matrices M which satisfy symplectic conditions form a symplectic group. The symplectic conditions are equivalent with indirect conditions as they both lead to the equation \dot{\varepsilon}= J \nabla_\varepsilon H , which is used in both of the derivations. Invariance of the Poisson bracket The Poisson bracket which is defined as:\{u, v\}_\eta := \sum_{i=1}^{n} \left( \frac{\partial u}{\partial q_{i}} \frac{\partial v}{\partial p_{i}} - \frac{\partial u}{\partial p_i} \frac{\partial v}{\partial q_i}\right)can be represented in matrix form as: \{u, v\}_\eta := (\nabla_\eta u)^T J (\nabla_\eta v) Hence using partial derivative relations and symplectic condition gives:\{u, v\}_\eta = (\nabla_\eta u)^T J (\nabla_\eta v) = (M^T \nabla_\varepsilon u)^T J (M^T \nabla_\varepsilon v) = (\nabla_\varepsilon u)^T M J M^T (\nabla_\varepsilon v) = (\nabla_\varepsilon u)^T J (\nabla_\varepsilon v) = \{u, v\}_\varepsilon The symplectic condition can also be recovered by taking u=\varepsilon_i and v=\varepsilon_j which shows that (M J M^T )_{ij}= J_{i j} . Thus these conditions are equivalent to symplectic conditions. Furthermore, it can be seen that \mathcal P_{ij}(\varepsilon) = \{ \varepsilon_i,\varepsilon_j\}_\eta =(M J M^T )_{ij} , which is also the result of explicitly calculating the matrix element by expanding it. d \varepsilon=( dq_1, dp_{1},0,0,\ldots),\quad\delta \varepsilon=(\delta q_{1},\delta p_{1},0,0,\ldots). The area of the infinitesimal parallelogram is given by: \delta a(12)=d q_{1}\delta p_{1}-\delta q_{1} d p_{1}={(\delta\varepsilon)}^T\,J \, d \varepsilon. It follows from the M^T J M = J symplectic condition that the infinitesimal area is conserved under canonical transformation: \delta a(12)={(\delta\varepsilon)}^T\,J \,d \varepsilon={(M\delta\eta)}^T\,J \,Md \eta= {(\delta\eta)}^T\,M^TJM \,d \eta = {(\delta\eta)}^T\,J \,d\eta = \delta A(12). Note that the new coordinates need not be completely oriented in one coordinate momentum plane. Hence, the condition is more generally stated as an invariance of the form {(d\varepsilon)}^T\,J \, \delta \varepsilon under canonical transformation, expanded as: \sum \delta q \cdot dp - \delta p \cdot dq = \sum \delta Q \cdot dP - \delta P \cdot dQ If the above is obeyed for any arbitrary variations, it would be only possible if the indirect conditions are met. The form of the equation, {v}^T\,J \, w is also known as a symplectic product of the vectors {v} and w and the bilinear invariance condition can be stated as a local conservation of the symplectic product. == Liouville's theorem ==

The indirect conditions allow us to prove Liouville's theorem, which states that the volume in phase space is conserved under canonical transformations, i.e., \int \mathrm{d}\mathbf{q}\, \mathrm{d}\mathbf{p} = \int \mathrm{d}\mathbf{Q}\, \mathrm{d}\mathbf{P} By calculus, the latter integral must equal the former times the determinant of Jacobian \int \mathrm{d}\mathbf{Q}\, \mathrm{d}\mathbf{P} = \int \det (M) \, \mathrm{d}\mathbf{q}\, \mathrm{d}\mathbf{p} Where M := \frac{\partial (\mathbf{Q}, \mathbf{P})}{\partial (\mathbf{q}, \mathbf{p})} Exploiting the "division" property of Jacobians yields M \equiv \frac{\partial (\mathbf{Q}, \mathbf{P})}{\partial (\mathbf{q}, \mathbf{P})} \left/ \frac{\partial (\mathbf{q}, \mathbf{p})}{\partial (\mathbf{q}, \mathbf{P})} \right. Eliminating the repeated variables givesM \equiv \frac{\partial (\mathbf{Q})}{\partial (\mathbf{q})} \left/ \frac{\partial (\mathbf{p})}{\partial (\mathbf{P})} \right. Application of the indirect conditions above yields {{math|1=\operatorname{det}(M)=1}}. ==Generating function approach==

To guarantee a valid transformation between and , we may resort to a direct generating function approach. Both sets of variables must obey Hamilton's principle. That is the action integral over the Lagrangians \mathcal{L}_{qp}=\mathbf{p} \cdot \dot{\mathbf{q}} - H(\mathbf{q}, \mathbf{p}, t) and \mathcal{L}_{QP}=\mathbf{P} \cdot \dot{\mathbf{Q}} - K(\mathbf{Q}, \mathbf{P}, t), obtained from the respective Hamiltonian via an "inverse" Legendre transformation, must be stationary in both cases (so that one can use the Euler–Lagrange equations to arrive at Hamiltonian equations of motion of the designated form; as it is shown for example here): \begin{align} \delta \int_{t_{1}}^{t_{2}} \left[ \mathbf{p} \cdot \dot{\mathbf{q}} - H(\mathbf{q}, \mathbf{p}, t) \right] dt &= 0 \\ \delta \int_{t_{1}}^{t_{2}} \left[ \mathbf{P} \cdot \dot{\mathbf{Q}} - K(\mathbf{Q}, \mathbf{P}, t) \right] dt &= 0 \end{align} One way for both variational integral equalities to be satisfied is to have \lambda \left[ \mathbf{p} \cdot \dot{\mathbf{q}} - H(\mathbf{q}, \mathbf{p}, t) \right] = \mathbf{P} \cdot \dot{\mathbf{Q}} - K(\mathbf{Q}, \mathbf{P}, t) + \frac{dG}{dt} Lagrangians are not unique: one can always multiply by a constant and add a total time derivative and yield the same equations of motion (as discussed on Wikibooks). In general, the scaling factor is set equal to one; canonical transformations for which are called extended canonical transformations. is kept, otherwise the problem would be rendered trivial and there would be not much freedom for the new canonical variables to differ from the old ones. Here is a generating function of one old canonical coordinate ( or ), one new canonical coordinate ( or ) and (possibly) the time . Thus, there are four basic types of generating functions (although mixtures of these four types can exist), depending on the choice of variables. As will be shown below, the generating function will define a transformation from old to new canonical coordinates, and any such transformation is guaranteed to be canonical. The various generating functions and its properties tabulated below is discussed in detail: Type 1 generating function The type 1 generating function depends only on the old and new generalized coordinates G \equiv G_{1}(\mathbf{q}, \mathbf{Q}, t). To derive the implicit transformation, we expand the defining equation above \mathbf{p} \cdot \dot{\mathbf{q}} - H(\mathbf{q}, \mathbf{p}, t) = \mathbf{P} \cdot \dot{\mathbf{Q}} - K(\mathbf{Q}, \mathbf{P}, t) + \frac{\partial G_{1}}{\partial t} + \frac{\partial G_{1}}{\partial \mathbf{q}} \cdot \dot{\mathbf{q}} + \frac{\partial G_{1}}{\partial \mathbf{Q}} \cdot \dot{\mathbf{Q}} Since the new and old coordinates are each independent, the following equations must hold \begin{align} \mathbf{p} &= \frac{\partial G_{1}}{\partial \mathbf{q}} \\ \mathbf{P} &= -\frac{\partial G_{1}}{\partial \mathbf{Q}} \\ K &= H + \frac{\partial G_{1}}{\partial t} \end{align} These equations define the transformation as follows: The first set of equations \ \mathbf{p} = \frac{\ \partial G_{1}\ }{ \partial \mathbf{q} }\ define relations between the new generalized coordinates and the old canonical coordinates . Ideally, one can invert these relations to obtain formulae for each as a function of the old canonical coordinates. Substitution of these formulae for the coordinates into the second set of equations \mathbf{P} = -\frac{\partial G_{1}}{\partial \mathbf{Q}} yields analogous formulae for the new generalized momenta in terms of the old canonical coordinates . We then invert both sets of formulae to obtain the old canonical coordinates as functions of the new canonical coordinates . Substitution of the inverted formulae into the final equation K = H + \frac{\partial G_{1}}{\partial t} yields a formula for as a function of the new canonical coordinates . In practice, this procedure is easier than it sounds, because the generating function is usually simple. For example, let G_{1} \equiv \mathbf{q} \cdot \mathbf{Q}. This results in swapping the generalized coordinates for the momenta and vice versa \begin{align} \mathbf{p} &= \frac{\partial G_{1}}{\partial \mathbf{q}} = \mathbf{Q} \\ \mathbf{P} &= -\frac{\partial G_{1}}{\partial \mathbf{Q}} = -\mathbf{q} \end{align} and . This example illustrates how independent the coordinates and momenta are in the Hamiltonian formulation; they are equivalent variables. Type 2 generating function The type 2 generating function G_{2}(\mathbf{q}, \mathbf{P}, t) depends only on the old generalized coordinates and the new generalized momenta G \equiv G_{2}(\mathbf{q}, \mathbf{P}, t)-\mathbf{Q} \cdot \mathbf{P} where the -\mathbf{Q} \cdot \mathbf{P} terms represent a Legendre transformation to change the right-hand side of the equation below. To derive the implicit transformation, we expand the defining equation above \mathbf{p} \cdot \dot{\mathbf{q}} - H(\mathbf{q}, \mathbf{p}, t) = -\mathbf{Q} \cdot \dot{\mathbf{P}} - K(\mathbf{Q}, \mathbf{P}, t) + \frac{\partial G_{2}}{\partial t} + \frac{\partial G_{2}}{\partial \mathbf{q}} \cdot \dot{\mathbf{q}} + \frac{\partial G_{2}}{\partial \mathbf{P}} \cdot \dot{\mathbf{P}} Since the old coordinates and new momenta are each independent, the following equations must hold \begin{align} \mathbf{p} &= \frac{\partial G_{2}}{\partial \mathbf{q}} \\ \mathbf{Q} &= \frac{\partial G_{2}}{\partial \mathbf{P}} \\ K &= H + \frac{\partial G_{2}}{\partial t} \end{align} These equations define the transformation as follows: The first set of equations \mathbf{p} = \frac{\partial G_{2}}{\partial \mathbf{q}} define relations between the new generalized momenta and the old canonical coordinates . Ideally, one can invert these relations to obtain formulae for each as a function of the old canonical coordinates. Substitution of these formulae for the coordinates into the second set of equations \mathbf{Q} = \frac{\partial G_{2}}{\partial \mathbf{P}} yields analogous formulae for the new generalized coordinates in terms of the old canonical coordinates . We then invert both sets of formulae to obtain the old canonical coordinates as functions of the new canonical coordinates . Substitution of the inverted formulae into the final equation K = H + \frac{\partial G_{2}}{\partial t} yields a formula for as a function of the new canonical coordinates . In practice, this procedure is easier than it sounds, because the generating function is usually simple. For example, let G_{2} \equiv \mathbf{g}(\mathbf{q}; t) \cdot \mathbf{P} where is a set of functions. This results in a point transformation of the generalized coordinates \mathbf{Q} = \frac{\partial G_{2}}{\partial \mathbf{P}} = \mathbf{g}(\mathbf{q}; t). Type 3 generating function The type 3 generating function G_{3}(\mathbf{p}, \mathbf{Q}, t) depends only on the old generalized momenta and the new generalized coordinates G \equiv G_{3}(\mathbf{p}, \mathbf{Q}, t)+ \mathbf{q} \cdot \mathbf{p} where the \mathbf{q} \cdot \mathbf{p} terms represent a Legendre transformation to change the left-hand side of the equation below. To derive the implicit transformation, we expand the defining equation above -\mathbf{q} \cdot \dot{\mathbf{p}} - H(\mathbf{q}, \mathbf{p}, t) = \mathbf{P} \cdot \dot{\mathbf{Q}} - K(\mathbf{Q}, \mathbf{P}, t) + \frac{\partial G_{3}}{\partial t} + \frac{\partial G_{3}}{\partial \mathbf{p}} \cdot \dot{\mathbf{p}} + \frac{\partial G_{3}}{\partial \mathbf{Q}} \cdot \dot{\mathbf{Q}} Since the new and old coordinates are each independent, the following equations must hold \begin{align} \mathbf{q} &= -\frac{\partial G_{3}}{\partial \mathbf{p}} \\ \mathbf{P} &= -\frac{\partial G_{3}}{\partial \mathbf{Q}} \\ K &= H + \frac{\partial G_{3}}{\partial t} \end{align} These equations define the transformation as follows: The first set of equations \mathbf{q} = -\frac{\partial G_{3}}{\partial \mathbf{p}} define relations between the new generalized coordinates and the old canonical coordinates . Ideally, one can invert these relations to obtain formulae for each as a function of the old canonical coordinates. Substitution of these formulae for the coordinates into the second set of equations \mathbf{P} = -\frac{\partial G_{3}}{\partial \mathbf{Q}} yields analogous formulae for the new generalized momenta in terms of the old canonical coordinates . We then invert both sets of formulae to obtain the old canonical coordinates as functions of the new canonical coordinates . Substitution of the inverted formulae into the final equation K = H + \frac{\partial G_{3}}{\partial t} yields a formula for as a function of the new canonical coordinates . In practice, this procedure is easier than it sounds, because the generating function is usually simple. Type 4 generating function The type 4 generating function G_{4}(\mathbf{p}, \mathbf{P}, t) depends only on the old and new generalized momenta G \equiv G_{4}(\mathbf{p}, \mathbf{P}, t) +\mathbf{q} \cdot \mathbf{p} - \mathbf{Q} \cdot \mathbf{P} where the \mathbf{q} \cdot \mathbf{p} - \mathbf{Q} \cdot \mathbf{P} terms represent a Legendre transformation to change both sides of the equation below. To derive the implicit transformation, we expand the defining equation above -\mathbf{q} \cdot \dot{\mathbf{p}} - H(\mathbf{q}, \mathbf{p}, t) = -\mathbf{Q} \cdot \dot{\mathbf{P}} - K(\mathbf{Q}, \mathbf{P}, t) + \frac{\partial G_{4}}{\partial t} + \frac{\partial G_{4}}{\partial \mathbf{p}} \cdot \dot{\mathbf{p}} + \frac{\partial G_{4}}{\partial \mathbf{P}} \cdot \dot{\mathbf{P}} Since the new and old coordinates are each independent, the following equations must hold \begin{align} \mathbf{q} &= -\frac{\partial G_{4}}{\partial \mathbf{p}} \\ \mathbf{Q} &= \frac{\partial G_{4}}{\partial \mathbf{P}} \\ K &= H + \frac{\partial G_{4}}{\partial t} \end{align} These equations define the transformation as follows: The first set of equations \mathbf{q} = -\frac{\partial G_{4}}{\partial \mathbf{p}} define relations between the new generalized momenta and the old canonical coordinates . Ideally, one can invert these relations to obtain formulae for each as a function of the old canonical coordinates. Substitution of these formulae for the coordinates into the second set of equations \mathbf{Q} = \frac{\partial G_{4}}{\partial \mathbf{P}} yields analogous formulae for the new generalized coordinates in terms of the old canonical coordinates . We then invert both sets of formulae to obtain the old canonical coordinates as functions of the new canonical coordinates . Substitution of the inverted formulae into the final equation K = H + \frac{\partial G_{4}}{\partial t} yields a formula for as a function of the new canonical coordinates . Limitations on the four types of generating functions Considering G_{2}(\mathbf{q}, \mathbf{P}, t) as an example, using generating function of second kind: {p}_i = \frac{\partial G_{2}}{\partial {q}_i} and {Q}_i = \frac{\partial G_{2}}{\partial {P}_i} , the first set of equations consisting of variables \mathbf{p} , \mathbf{q} and \mathbf{P} has to be inverted to get \mathbf{P}(\mathbf q, \mathbf p) . This process is possible when the matrix defined by a_{ij}=\frac{\partial {p}_i(\mathbf q,\mathbf P)}{\partial P_j} is non-singular using the inverse function theorem, and can be restated as the following relation. \left|\begin{array}{l l l}{{\displaystyle{\frac{\partial^{2}G_{2}}{\partial P_{1}\partial q_{1}}}}}&&{{\displaystyle{\frac{\partial^{2}G_{2}}{\partial P_{1}\partial q_{n}}}}}\\ {\quad \vdots} & {\ddots}&{\quad \vdots}\\{{\displaystyle{\frac{\partial^{2}G_{2}}{\partial P_{n}\partial q_{1}}}}}&&{{\displaystyle{\frac{\partial^{2}G_{2}}{\partial P_{n}\partial q_{n}}}}}\end{array}\right|{\neq0} Hence, restrictions are placed on generating functions to have the matrices: \left[\frac{\partial^2 G_1}{\partial Q_j\partial q_i} \right] , \left[\frac{\partial^2 G_2}{\partial P_j\partial q_i} \right] , \left[\frac{\partial^2 G_3}{\partial p_j\partial Q_i} \right] and \left[\frac{\partial^2 G_4}{\partial p_j\partial P_i} \right] , being non-singular. These conditions also correspond to local invertibility of the coordinates. From these restrictions, it can be stated that type 1 and type 4 generating functions always have a non-singular \left[\frac{\partial Q_i(\mathbf q,\mathbf p)}{\partial p_j} \right] matrix whereas type 2 and type 3 generating functions always have a non-singular \left[\frac{\partial P_i(\mathbf q,\mathbf p)}{\partial p_j} \right] matrix. Hence, the canonical transformations resulting from these four generating functions alone are not completely general. Generalized use of generating functions In other words, since and are each independent functions, it follows that to have generating function of the form G_{1}(\mathbf{q}, \mathbf{Q}, t) and G_{4}(\mathbf{p}, \mathbf{P}, t) or G_{2}(\mathbf{q}, \mathbf{P}, t) and G_{3}(\mathbf{p}, \mathbf{Q}, t), the corresponding Jacobian matrices \left[\frac{\partial Q_i}{\partial p_j} \right] and \left[\frac{\partial P_i}{\partial p_j} \right] are restricted to be non singular, ensuring that the generating function is a function of independent variables. However, as a feature of canonical transformations, it is always possible to choose such independent functions from sets or , to form a generating function representation of canonical transformations, including the time variable. Hence, it can be proven that every finite canonical transformation can be given as a closed but implicit form that is a variant of the given four simple forms. == Canonical transformation conditions ==

Canonical transformation relations From: K = H + \frac{\partial G}{\partial t} , calculate \frac{\partial (K-H)}{\partial P} : \begin{align} \left( \frac{\partial (K-H)}{\partial P}\right)_{Q,P,t} &= \frac{\partial K}{\partial P} - \frac{\partial H}{\partial p}\frac{\partial p}{\partial P} - \frac{\partial H}{\partial q}\frac{\partial q}{\partial P} - \frac{\partial H}{\partial t}\left( \frac{\partial t}{\partial P}\right)_{Q,P,t} \\ &= \dot{Q} + \dot{p} \frac{\partial q}{\partial P} - \dot{q}\frac{\partial p}{\partial P} \\ &= \frac{\partial Q}{\partial t} + \frac{\partial Q}{\partial q} \cdot \dot{q} + \frac{\partial Q}{\partial p} \cdot \dot{p} + \dot{p} \frac{\partial q}{\partial P} - \dot{q}\frac{\partial p}{\partial P} \\ &=\dot{q}\left(\frac{\partial Q}{\partial q} - \frac{\partial p}{\partial P}\right)+\dot{p}\left(\frac{\partial q}{\partial P} +\frac{\partial Q}{\partial p} \right) + \frac{\partial Q}{\partial t} \end{align} Since the left hand side is \frac{\partial (K-H)}{\partial P} = \frac \partial {\partial P}\left( \frac{\partial G}{\partial t} \right) \bigg |_{Q,P,t} which is independent of dynamics of the particles, equating coefficients of \dot q and \dot p to zero, canonical transformation rules are obtained. This step is equivalent to equating the left hand side as \frac{\partial (K-H)}{\partial P} = \frac{\partial Q}{\partial t} . Since the left hand side is \frac{\partial (K-H)}{\partial P} = \frac \partial {\partial P}\left( \frac{\partial G}{\partial t} \right) \bigg |_{Q,P,t} which is independent of dynamics of the particles, equating coefficients of \dot q and \dot p to zero, canonical transformation rules are obtained. This step is equivalent to equating the left hand side as \frac{\partial (K-H)}{\partial P} = \frac{\partial Q}{\partial t} . Similarly: \begin{align} \left(\frac{\partial (K-H)}{\partial Q}\right)_{Q,P,t} &= \frac{\partial K}{\partial Q} - \frac{\partial H}{\partial p}\frac{\partial p}{\partial Q} - \frac{\partial H}{\partial q}\frac{\partial q}{\partial Q} - \frac{\partial H}{\partial t}\left(\frac{\partial t}{\partial Q}\right)_{Q,P,t} \\ &= -\dot{P} + \dot{p} \frac{\partial q}{\partial Q} - \dot{q}\frac{\partial p}{\partial Q} \\ &= -\frac{\partial P}{\partial t} -\frac{\partial P}{\partial q} \cdot \dot{q} - \frac{\partial P}{\partial p} \cdot \dot{p} + \dot{p} \frac{\partial q}{\partial Q} - \dot{q}\frac{\partial p}{\partial Q} \\ &=-\left(\dot{q}\left(\frac{\partial P}{\partial q} + \frac{\partial p}{\partial Q}\right)+\dot{p}\left(\frac{\partial P}{\partial p} -\frac{\partial q}{\partial Q} \right) + \frac{\partial P}{\partial t} \right) \end{align} Similarly the canonical transformation rules are obtained by equating the left hand side as \frac{\partial (K-H)}{\partial Q} = - \frac{\partial P}{\partial t} . The above two relations can be combined in matrix form as: J \left(\nabla_\varepsilon \frac{\partial G}{\partial t} \right) = \frac{\partial \varepsilon}{\partial t} (which will also retain same form for extended canonical transformation) where the result \frac{\partial G}{\partial t} = K-H , has been used. The canonical transformation relations are hence said to be equivalent to J \left(\nabla_\varepsilon \frac{\partial G}{\partial t} \right) = \frac{\partial \varepsilon}{\partial t} in this context. The canonical transformation relations can now be restated to include time dependence: \begin{align} \left( \frac{\partial Q_{m}}{\partial p_{n}}\right)_{\mathbf{q}, \mathbf{p},t} &= - \left( \frac{\partial q_{n}}{\partial P_{m}}\right)_{\mathbf{Q}, \mathbf{P},t} \\ \left( \frac{\partial Q_{m}}{\partial q_{n}}\right)_{\mathbf{q}, \mathbf{p},t} &= \left( \frac{\partial p_{n}}{\partial P_{m}}\right)_{\mathbf{Q}, \mathbf{P},t} \end{align} \begin{align} \left( \frac{\partial P_{m}}{\partial p_{n}}\right)_{\mathbf{q}, \mathbf{p},t} &= \left( \frac{\partial q_{n}}{\partial Q_{m}}\right)_{\mathbf{Q}, \mathbf{P},t} \\ \left( \frac{\partial P_{m}}{\partial q_{n}}\right)_{\mathbf{q}, \mathbf{p},t} &= - \left( \frac{\partial p_{n}}{\partial Q_{m}}\right)_{\mathbf{Q}, \mathbf{P},t} \end{align} Since \frac{\partial (K-H)}{\partial P} = \frac{\partial Q}{\partial t} and \frac{\partial (K-H)}{\partial Q} = - \frac{\partial P}{\partial t} , if and do not explicitly depend on time, K= H + \frac{\partial G}{\partial t}(t) can be taken. The analysis of restricted canonical transformations is hence consistent with this generalization. Symplectic condition Applying transformation of coordinates formula for \nabla_\eta H = M^T \nabla_\varepsilon H , in Hamiltonian's equations gives: \dot{\eta}=J\nabla_\eta H =J ( M^T \nabla_\varepsilon H) Similarly for \dot{\varepsilon} : \dot{\varepsilon}=M\dot{\eta} + \frac{\partial \varepsilon}{\partial t} =M J M^T \nabla_\varepsilon H + \frac{\partial \varepsilon}{\partial t} or: \dot{\varepsilon}=J \nabla_\varepsilon K = J \nabla_\varepsilon H + J \nabla_\varepsilon \left( \frac{\partial G}{\partial t}\right) Where the last terms of each equation cancel due to J \left(\nabla_\varepsilon \frac{\partial G}{\partial t} \right) = \frac{\partial \varepsilon}{\partial t} condition from canonical transformations. Hence leaving the symplectic relation: M J M^T = J which is also equivalent with the condition M^T J M = J . It follows from the above two equations that the symplectic condition implies the equation J \left(\nabla_\varepsilon \frac{\partial G}{\partial t} \right) = \frac{\partial \varepsilon}{\partial t} , from which the indirect conditions can be recovered. Thus, symplectic conditions and indirect conditions can be said to be equivalent in the context of using generating functions. Invariance of the Poisson and Lagrange brackets Since \mathcal P_{ij}(\varepsilon) = \{ \varepsilon_i,\varepsilon_j\}_\eta =(M J M^T )_{ij} = J_{ij} and \mathcal L_{ij}(\eta) =[\eta_i,\eta_j]_\varepsilon=(M^T J M )_{ij} = J_{ij} where the symplectic condition is used in the last equalities. Using \{\varepsilon_i,\varepsilon_j\}_\varepsilon=[\eta_i,\eta_j]_\eta = J_{ij} , the equalities \{ \varepsilon_i,\varepsilon_j\}_\eta= \{ \varepsilon_i,\varepsilon_j\}_\varepsilon and [\eta_i,\eta_j]_\varepsilon= [\eta_i,\eta_j]_\eta are obtained which imply the invariance of Poisson and Lagrange brackets. == Extended canonical transformation ==

Canonical transformation relations By solving for: \lambda \left[ \mathbf{p} \cdot \dot{\mathbf{q}} - H(\mathbf{q}, \mathbf{p}, t) \right] = \mathbf{P} \cdot \dot{\mathbf{Q}} - K(\mathbf{Q}, \mathbf{P}, t) + \frac{dG}{dt} with various forms of generating function, the relation between K and H goes as \frac{\partial G}{\partial t} = K-\lambda H instead, which also applies for \lambda = 1 case. All results presented below can also be obtained by replacing q \rightarrow \sqrt{\lambda}q , p \rightarrow \sqrt{\lambda}p and H \rightarrow {\lambda}H from known solutions, since it retains the form of Hamilton's equations. The extended canonical transformations are hence said to be result of a canonical transformation (\lambda = 1 ) and a trivial canonical transformation (\lambda \neq 1 ) which has M J M^T = \lambda J (for the given example, M = \sqrt{\lambda} I which satisfies the condition). Using same steps previously used in previous generalization, with \frac{\partial G}{\partial t} = K-\lambda H in the general case, and retaining the equation J \left(\nabla_\varepsilon \frac{\partial g}{\partial t} \right) = \frac{\partial \varepsilon}{\partial t} , extended canonical transformation partial differential relations are obtained as: \begin{align} \left( \frac{\partial Q_{m}}{\partial p_{n}}\right)_{\mathbf{q}, \mathbf{p},t} &= -\lambda \left( \frac{\partial q_{n}}{\partial P_{m}}\right)_{\mathbf{Q}, \mathbf{P},t} \\ \left( \frac{\partial Q_{m}}{\partial q_{n}}\right)_{\mathbf{q}, \mathbf{p},t} &= \lambda \left( \frac{\partial p_{n}}{\partial P_{m}}\right)_{\mathbf{Q}, \mathbf{P},t} \end{align} \begin{align} \left( \frac{\partial P_{m}}{\partial p_{n}}\right)_{\mathbf{q}, \mathbf{p},t} &= \lambda \left( \frac{\partial q_{n}}{\partial Q_{m}}\right)_{\mathbf{Q}, \mathbf{P},t} \\ \left( \frac{\partial P_{m}}{\partial q_{n}}\right)_{\mathbf{q}, \mathbf{p},t} &= -\lambda \left( \frac{\partial p_{n}}{\partial Q_{m}}\right)_{\mathbf{Q}, \mathbf{P},t} \end{align} Symplectic condition Following the same steps to derive the symplectic conditions, as: \dot{\eta}=J\nabla_\eta H =J ( M^T \nabla_\varepsilon H) and \dot{\varepsilon}=M\dot{\eta} + \frac{\partial \varepsilon}{\partial t} =M J M^T \nabla_\varepsilon H + \frac{\partial \varepsilon}{\partial t} where using \frac{\partial G}{\partial t} = K-\lambda H instead gives: \dot{\varepsilon}=J \nabla_\varepsilon K = \lambda J \nabla_\varepsilon H + J \nabla_\varepsilon \left( \frac{\partial G}{\partial t}\right) The second part of each equation cancel. Hence the condition for extended canonical transformation instead becomes: M J M^T = \lambda J . Poisson and Lagrange brackets The Poisson brackets are changed as follows: \{u, v\}_\eta = (\nabla_\eta u)^T J (\nabla_\eta v) = (M^T \nabla_\varepsilon u)^T J (M^T \nabla_\varepsilon v) = (\nabla_\varepsilon u)^T M J M^T (\nabla_\varepsilon v) = \lambda (\nabla_\varepsilon u)^T J (\nabla_\varepsilon v) = \lambda \{u, v\}_\varepsilon whereas, the Lagrange brackets are changed as: [u, v]_\varepsilon = (\partial_u \varepsilon )^T \,J\, (\partial_v \varepsilon) = (M \, \partial_u \eta )^T \,J \, ( M \,\partial_v \eta) = (\partial_u \eta )^T\, M^TJ M\, (\partial_v \eta) = \lambda (\partial_u \eta )^T\, J\,(\partial_v \eta) = \lambda [u, v]_\eta Hence, the Poisson bracket scales by the inverse of \lambda whereas the Lagrange bracket scales by a factor of \lambda . == Infinitesimal canonical transformation ==

Consider the canonical transformation that depends on a continuous parameter \alpha , as follows: \begin{align} & Q(q,p,t;\alpha) \quad \quad \quad & Q(q,p,t;0)=q \\ & P(q,p,t;\alpha) \quad \quad \text{with} \quad & P(q,p,t;0)=p \\ \end{align} For infinitesimal values of \alpha , the corresponding transformations are called as infinitesimal canonical transformations which are also known as differential canonical transformations. Explicit construction Consider the following generating function: G_2(q,P,t)= qP + \alpha G(q,P,t) Since for \alpha=0 , G_2 = qP has the resulting canonical transformation, Q = q and P = p , this type of generating function can be used for infinitesimal canonical transformation by restricting \alpha to an infinitesimal value. From the conditions of generators of second type: \begin{align} {p} &= \frac{\partial G_{2}}{\partial {q}} = P + \alpha \frac{\partial G}{\partial {q}} (q,P,t) \\ {Q} &= \frac{\partial G_{2}}{\partial {P}} = q + \alpha \frac{\partial G}{\partial {P}} (q,P,t) \\ \end{align} Since P = P(q,p,t;\alpha) , changing the variables of the function G to G(q,p,t) and neglecting terms of higher order of \alpha , gives: \begin{align} {p} &= P + \alpha \frac{\partial G}{\partial {q}} (q,p,t) \\ {Q} &= q + \alpha \frac{\partial G}{\partial p} (q,p,t) \\ \end{align} Infinitesimal canonical transformations can also be derived using the matrix form of the symplectic condition. The function G(q,p,t) is very significant in infinitesimal canonical transformations and is referred to as the generator of infinitesimal canonical transformation. Active and passive transformations In the active view of transformations, the coordinate system is changed without the physical system changing, whereas in the passive view of transformation, the coordinate system is retained and the physical system is said to undergo transformations. Active view of transformation Thus, using the relations from infinitesimal canonical transformations, the change in the system states under active view of the canonical transformation is said to be: \begin{align} & \delta q = \alpha \frac{\partial G}{\partial p} (q,p,t) \quad \text{and} \quad \delta p = - \alpha \frac{\partial G}{\partial q} (q,p,t) , \\ \end{align} or as \delta \eta = \alpha J \nabla_\eta G in matrix form. For any function u(\eta) , it changes under active view of the transformation according to: \delta u = u(\eta +\delta \eta)-u(\eta) = (\nabla_\eta u)^T\delta\eta=\alpha (\nabla_\eta u)^T J (\nabla_\eta G) = \alpha \{ u,G \} . Passive view of transformation Considering the change of Hamiltonians in the passive view, i.e., for a fixed point,K(Q=q_0,P=p_0,t) - H(q=q_0,p=p_0,t) = \left(H(q_0',p_0',t) + \frac{\partial G_{2}}{\partial t}\right) - H(q_0,p_0,t) = - \delta H +\alpha \frac{\partial G}{\partial t} = \alpha\left(\{ G,H\}+\frac{\partial G}{\partial t} \right)=\alpha\frac{dG}{dt} where (q=q_0',p=p_0') are mapped to the point, (Q=q_0,P=p_0) by the infinitesimal canonical transformation, and similar change of variables for G(q,P,t) to G(q,p,t) is considered up-to first order of \alpha . Hence, if the Hamiltonian is invariant for infinitesimal canonical transformations, its generator is a constant of motion. Generators of dynamical symmetry transformations Consider the transformation where the change of coordinates also depends on the generalized velocities. \begin{align} q^r\to q^r+\delta q^r\\ \delta q^r=\epsilon\phi^r(q,\dot{q},t)\\ \end{align} If the above is a dynamical symmetry, then the lagrangian changes by: \delta L=\epsilon\frac d {dt}F(q,\dot q,t) and the new Lagrangian is said to be dynamically equivalent to the old Lagrangian as it ensures the resultant equations of motion being the same. The change in generalized velocity and momentum term can be derived as: \begin{align} p=\frac{\partial L}{\partial \dot q}, \quad& \dot q=\frac {dq}{dt}\\ \delta p_r=\frac{\partial^2L}{\partial q^s\partial\dot q^r}\delta q^s+\frac{\partial^2 L}{\partial \dot q^s\partial \dot q^r}\delta \dot q^s,\quad&\delta \dot q^r=\epsilon \frac{\partial \phi^r}{\partial q^s} \dot q^s+\epsilon \frac{\partial \phi^r}{\partial \dot q^s}\ddot q^s+\epsilon\frac{\partial\phi^r}{\partial t} \\ \end{align} Generator of transformation Using the change in Lagrangian property of a dynamical symmetry: \frac d{dt}F=\frac{\partial F}{\partial q^r}\dot q^r+\frac{\partial F}{\partial \dot q^r}\ddot q^r+\frac{\partial F}{\partial t}=\frac{\delta L}{\epsilon}=\left(\frac{\partial L}{\partial q^r}\phi^r+\frac{\partial L}{\partial \dot q^r}\frac{\partial \phi^r}{\partial t}\right)+p_s\frac{\partial \phi^s}{\partial q^r}\dot q^r+p_s\frac{\partial \phi^s}{\partial \dot q^r}\ddot q^r Since the \ddot q terms appear only once in either side and the equation must hold independent of dynamics or equation of motion that relate \ddot q to (q,\dot q,t), it's coefficients must be equal for this to be true, giving the relation: p_s\frac{\partial \phi^s}{\partial \dot q^r}=\frac{\partial F}{\partial \dot q^r} using which, it can be shown that \{q^r,\epsilon (p_s\phi^s-F)\}=\delta q^r,\quad \{p_r,\epsilon(p_s\phi^s-F)\}=\delta p_r+\epsilon\left(\frac{\partial L}{\partial q^s}-\frac{d}{dt}\frac{\partial L}{\partial \dot q^s}\right)\frac{\partial \phi^s}{\partial \dot q^r} Hence, the term p\phi-F generates the canonical dynamical symmetry transformation if either the Euler Lagrange relation gives zero, or if \frac{\partial \phi_s}{\partial \dot q^r}=0\,\forall s,r which is a infinitesimal point transformation. Note that in the point transformation condition, the quantity generates the transformation regardless of if the Euler Lagrange equations are satisfied and since they do not depend on the dynamics of the problem are said to be a purely kinematic relation. Similar results are obtained in classical field theory, for example, in a Lorentz invariant Lagrangian density where corresponding conserved charges, momentum density P^\mu generates translation of fields and M^{\mu\nu}of Lorentz invariance generates Lorentz transformation of fields. Noether Invariant Using Euler Lagrange relation for the provided Lagrangian, the invariants of motion can be derived as:\delta L-\epsilon\frac d {dt}F(q,\dot q,t)= \epsilon\phi\cancelto{=0}{\left(\frac{\partial}{\partial q}-\frac{d}{dt}\frac{\partial}{\partial \dot q}\right)L}+\epsilon\frac{d}{dt}\left(\phi\frac{\partial}{\partial \dot q}L- F\right)=\epsilon\frac{d}{dt}\left(\phi\frac{\partial}{\partial \dot q}L- F\right)=0 Hence \left(\phi\frac{\partial}{\partial \dot q}L-F\right)=p\phi-F is a constant of motion. Hence, the derived Noether invariant also generates the same symmetry transformation as shown previously. Examples of ICT Time evolution Taking G(q,p,t)=H(q,p,t) and \alpha = dt , then \delta \eta = (J \nabla_\eta H) dt = \dot{\eta} dt = d\eta . Thus the continuous application of such a transformation maps the coordinates \eta(\tau) to \eta(\tau+t) . Hence if the Hamiltonian is time translation invariant, i.e. does not have explicit time dependence, its value is conserved for the motion. Translation Taking G(q,p,t)=p_k , \delta p_i = 0 and \delta q_i = \alpha \delta_{ik} . Hence, the canonical momentum generates a shift in the corresponding generalized coordinate and if the Hamiltonian is invariant of translation, the momentum is a constant of motion. Rotation Consider an orthogonal system for an N-particle system: \begin{array}{l}{{\mathbf q=\left(x_{1},y_{1},z_{1},\ldots,x_{n},y_{n},z_{n}\right),}}\\ {{\mathbf p=\left(p_{1x},p_{1y},p_{1z},\ldots,p_{n x},p_{n y},p_{n z}\right).}}\end{array} Choosing the generator to be: G=L_{z}=\sum_{i=1}^{n}\left(x_{i}p_{i y}-y_{i}p_{i x}\right) and the infinitesimal value of \alpha = \delta \phi , then the change in the coordinates is given for x by: \begin{array}{c} {\delta x_{i}=\{x_{i},G\}\delta\phi=\displaystyle\sum_{j} \{x_{i},x_{j}p_{j y}-y_{j}p_{j x}\}\delta\phi=\displaystyle\sum_{j}(\underbrace{\{x_{i},x_{j}p_{j y}\}}_{=0} -{ \{x_{i},y_{j}p_{j x}\}}})\delta\phi\\ {{=\displaystyle -\sum_{j} y_{j} \underbrace{\{x_i,p_{jx}\}}_{=\delta_{ij}}\delta\phi=- y_{i} \delta \phi}} \end{array} and similarly for y: \begin{array}{c} \delta y_{i}=\{y_{i},G\}\delta\phi=\displaystyle\sum_{j}\{y_{i},x_{j}p_{j y}-y_{j}p_{j x}\}\delta\phi=\displaystyle\sum_{j}(\{y_{i},x_{j}p_{j y}\}-\underbrace{ \{y_{i},y_{j}p_{j x}\}}_{=0})\delta \phi\\ {=\displaystyle\sum_{j}x_{j}\underbrace{\{y_i,p_{jy}\}}_{=\delta_{ij}} \delta\phi=x_{i}\delta\phi\,,} \end{array} whereas the z component of all particles is unchanged: \delta z_{ i }=\left\{z_{i},G\right\}\delta\phi=\sum_{j}\left\{z_{i},x_{j}p_{j y}-y_{j}p_{j x}\right\}\delta \phi =0. These transformations correspond to rotation about the z axis by angle \delta \phi in its first order approximation. Hence, repeated application of the infinitesimal canonical transformation generates a rotation of system of particles about the z axis. If the Hamiltonian is invariant under rotation about the z axis, the generator, the component of angular momentum along the axis of rotation, is an invariant of motion. == One parameter subgroup of Canonical transformations ==

Allowing the values of \alpha to take continuous range of values in: \begin{align} & Q(q,p,t;\alpha) \quad \quad \quad & Q(q,p,t;0)=q \\ & P(q,p,t;\alpha) \quad \quad \text{with} \quad & P(q,p,t;0)=p \\ \end{align} which can be expressed as \epsilon^\mu(\eta,t;\alpha ) where \epsilon^\mu(\eta,t;0)=\eta^\mu . One parameter subgroup of Canonical transformations are those where the generator of the transformation can be used to generate coordinates where\epsilon^\mu(\epsilon(\eta,t;\alpha_1);\alpha_2)=\epsilon^\mu(\eta,t;\alpha_1+\alpha_2) is satisfied, i.e. composition of two canonical transformations of parameter \alpha_1 and \alpha_2 are the same as that of a single canonical transformation of parameter \alpha_1+\alpha_2 . The condition on the transformations of the one parameter subgroup kind can be expressed equivalently as a differential equation: \delta\epsilon^\mu(\eta,t;\alpha)=\delta\alpha\{\epsilon^\nu,G \}=\delta\alpha J^{\mu\nu}\frac{\partial G}{\partial \epsilon^\nu}(\epsilon(\eta,t;\alpha ),t) \implies \frac{d\epsilon^\mu(\eta,t;\alpha)}{d \alpha}= J^{\mu\nu}\frac{\partial G}{\partial \epsilon^\nu}(\epsilon(\eta,t;\alpha ),t) for all \eta given that the generator has no explicit dependence on \alpha . The conditions \epsilon^\mu(\epsilon(\eta,t;\alpha_1);\alpha_2)=\epsilon^\mu(\eta,t;\alpha_1+\alpha_2) can be recovered since this equation is trivially satisfied when \alpha_2=0 which is considered initial values and the differential equations of both sides are of the same form implying the relation due to uniqueness of solutions with given initial values. Hence one parameter subgroups of canonical transformations are extension of infinitesimal canonical transformations to finite values of \alpha by using the same functional form of its generator independent of parameter \alpha . \epsilon(\eta,t;\alpha)=\eta+ \alpha\{\eta,G(\eta,t)\}+\frac{1}{2!}\alpha^2 \{\{\eta,G(\eta,t)\},G(\eta,t)\}+\cdots=e^{- \alpha \tilde G} \eta Change in function values \frac{df(\epsilon(\eta;\alpha),t)}{d \alpha}= \{f(\epsilon(\eta;\alpha),t),G(\eta,t)\}_\eta=:-\tilde G f(\epsilon(\eta;\alpha),t) by taking repeatedly in steps and using \epsilon(\eta,t;0)=\eta we get similarly f(e^{-\alpha\tilde G}\eta,t)=f(\epsilon(\eta;\alpha),t)=f(\eta,t)+ \alpha\{f(\eta,t),G(\eta,t)\}+\frac{1}{2!}\alpha^2 \{\{f(\eta,t),G(\eta,t)\},G(\eta,t)\}+\cdots=e^{- \alpha \tilde G} f(\eta,t) Passive view of transformation Change in a function can be invoked by preserving its values on the same physical states in phase space as f(\epsilon,t)=f(\epsilon(\eta;\alpha),t)=f'(\epsilon(\eta;\alpha+\delta\alpha),t)= f'(\epsilon',t) can be expressed as upto first order as: \delta' f=f'(\epsilon)-f(\epsilon)=f'(\epsilon)-f'(\epsilon')\approx f(\epsilon(\eta;\alpha-\delta\alpha))-f(\epsilon(\eta;\alpha)) =-\delta \alpha\{f,G\} Including the change in the function as some explicit dependence on parameter of transformation \alpha , it can be expressed as f(\epsilon,t;\alpha) where it is explicitly dependent on \alpha such that \frac{\partial f(\epsilon,t;\alpha)}{\partial \alpha} =-\{f,G\} which indicates that the function transforms oppositely to that due to the coordinates to preserve well defined mapping from a physical point in phase space to its scalar values. It is also possible that functions transform without needing to preserve its values on the same physical states in phase space. Such as, for example, the Hamiltonian whose explicit dependence on the canonical transformation can be different from the above form, restated from its previous derivation as \frac{\partial H(\epsilon,t;\alpha)}{\partial \alpha} =\frac{dG}{dt} which is similar to previous relation but also accounts for any explicit time dependence of the generator. Hence, if the Hamiltonian is invariant in passive view for infinitesimal canonical transformations, its generator is a constant of motion. == Motion as canonical transformation ==

Motion itself (or, equivalently, a shift in the time origin) is a canonical transformation. If \mathbf{Q}(t) \equiv \mathbf{q}(t+\tau) and \mathbf{P}(t) \equiv \mathbf{p}(t+\tau), then Hamilton's principle is automatically satisfied \delta \int_{t_1}^{t_2} \left[ \mathbf{P} \cdot \dot{\mathbf{Q}} - K(\mathbf{Q}, \mathbf{P}, t) \right] dt = \delta \int_{t_1 + \tau}^{t_2 + \tau} \left[ \mathbf{p} \cdot \dot{\mathbf{q}} - H(\mathbf{q}, \mathbf{p}, t+\tau) \right] dt = 0 since a valid trajectory (\mathbf{q}(t), \mathbf{p}(t)) should always satisfy Hamilton's principle, regardless of the endpoints. == Examples ==

• The translation \mathbf{Q}(\mathbf{q}, \mathbf{p})= \mathbf{q} + \mathbf{a}, \mathbf{P}(\mathbf{q}, \mathbf{p})= \mathbf{p} + \mathbf{b} where \mathbf{a}, \mathbf{b} are two constant vectors is a canonical transformation. Indeed, the Jacobian matrix is the identity, which is symplectic: I^\text{T}JI=J. • Set \mathbf{x}=(q,p) and \mathbf{X}=(Q,P), the transformation \mathbf{X}(\mathbf{x})=R \mathbf{x} where R \in SO(2) is a rotation matrix of order 2 is canonical. Keeping in mind that special orthogonal matrices obey R^\text{T}R=I it's easy to see that the Jacobian is symplectic. However, this example only works in dimension 2: SO(2) is the only special orthogonal group in which every matrix is symplectic. Note that the rotation here acts on (q,p) and not on q and p independently, so these are not the same as a physical rotation of an orthogonal spatial coordinate system. • The transformation (Q(q,p), P(q,p))=(q+f(p), p), where f(p) is an arbitrary function of p, is canonical. Jacobian matrix is indeed given by \frac{\partial X}{\partial x} = \begin{bmatrix} 1 & f'(p) \\ 0 & 1 \end{bmatrix} which is symplectic. ==Modern mathematical description==

In mathematical terms, canonical coordinates are any coordinates on the phase space (cotangent bundle) of the system that allow the canonical one-form to be written as \sum_i p_i\,dq^i up to a total differential (exact form). The change of variable between one set of canonical coordinates and another is a canonical transformation. The index of the generalized coordinates is written here as a superscript (q^{i}), not as a subscript as done above (q_{i}). The superscript conveys the contravariant transformation properties of the generalized coordinates, and does not mean that the coordinate is being raised to a power. Further details may be found at the symplectomorphism article. ==History==

The first major application of the canonical transformation was in 1846, by Charles Delaunay, in the study of the Earth-Moon-Sun system. This work resulted in the publication of a pair of large volumes as Mémoires by the French Academy of Sciences, in 1860 and 1867. ==See also==