The Christoffel Symbol

This Chapter is devoted to the all-important Christoffel symbol, an object that captures the variability of the covariant basis from one point to another in curvilinear coordinates. As such, it can be used to "subtract out" the adverse effects of that variability in various differential operators including the covariant derivative.
The covariant basis vectors Zi\mathbf{Z}_{i}, given by
Zi(Z)=R(Z)Zi,(9.9)\mathbf{Z}_{i}\left( Z\right) =\frac{\partial\mathbf{R}\left( Z\right) }{\partial Z^{i}}, \tag{9.9}
can be said to represent the rates of change of the position vector R\mathbf{R} with respect to each of the coordinates ZiZ^{i}. As a reminder, the symbols R(Z)\mathbf{R}\left( Z\right) and Zi(Z)\mathbf{Z}_{i}\left( Z\right) represent the functions R(Z1,Z2,Z3)\mathbf{R}\left( Z^{1},Z^{2} ,Z^{3}\right) and Zi(Z1,Z2,Z3)\mathbf{Z}_{i}\left( Z^{1},Z^{2},Z^{3}\right) , i.e. the position vector R\mathbf{R} and the covariant basis Zi\mathbf{Z}_{i} as functions of the coordinates ZiZ^{i}.
In addition to the ubiquitous covariant basis Zi\mathbf{Z}_{i}, we have, on a number of occasions, encountered the second-order system
Zi(Z)Zj(12.1)\frac{\partial\mathbf{Z}_{i}\left( Z\right) }{\partial Z^{j}}\tag{12.1}
that represents the rates of change of each of the covariant basis vectors Zi\mathbf{Z}_{i} with respect to each of the coordinates ZjZ^{j}. It is natural to use two subscripts to enumerate the elements of this system and we will therefore use the symbol Γij\mathbf{\Gamma}_{ij} to denote it, i.e.
Γij=Zi(Z)Zj.(12.2)\mathbf{\Gamma}_{ij}=\frac{\partial\mathbf{Z}_{i}\left( Z\right) }{\partial Z^{j}}.\tag{12.2}
Note that the symbol Γ\mathbf{\Gamma} is bold to indicate that the elements of Γij\mathbf{\Gamma}_{ij} are vectors.
The system Γij\mathbf{\Gamma}_{ij} can also be thought of as the collection of the second-order derivatives of the position vector R\mathbf{R} with respect to the coordinates:
Γij=2R(Z)ZiZj.(12.3)\mathbf{\Gamma}_{ij}=\frac{\partial^{2}\mathbf{R}\left( Z\right) }{\partial Z^{i}\partial Z^{j}}.\tag{12.3}
In the future, we will consider higher-order derivatives. The Christoffel symbol, however, is about the second order.
Since partial derivatives commute, i.e.
2R(Z)ZiZj=2R(Z)ZjZi,(12.4)\frac{\partial^{2}\mathbf{R}\left( Z\right) }{\partial Z^{i}\partial Z^{j} }=\frac{\partial^{2}\mathbf{R}\left( Z\right) }{\partial Z^{j}\partial Z^{i}},\tag{12.4}
Γij\mathbf{\Gamma}_{ij} is symmetric, i.e.
Γij=Γji,(12.5)\mathbf{\Gamma}_{ij}=\mathbf{\Gamma}_{ji},\tag{12.5}
or
Zi(Z)Zj=Zj(Z)Zi.(12.6)\frac{\partial\mathbf{Z}_{i}\left( Z\right) }{\partial Z^{j}}=\frac {\partial\mathbf{Z}_{j}\left( Z\right) }{\partial Z^{i}}.\tag{12.6}
In affine coordinates, the vectors Γij\mathbf{\Gamma}_{ij} vanish since the covariant basis is the same at all points. In all other coordinate systems, the covariant basis varies from one point to another and we can therefore expect Γij\mathbf{\Gamma}_{ij} to be nonzero. In the nn-dimensional space, the second-order system Γij\mathbf{\Gamma}_{ij} consists of n2n^{2} vectors. However, because of the aforementioned symmetry, only n(n+1)/2n\left( n+1\right) /2 vectors can be distinct: 66 in three dimensions, 33 in two dimensions, and 11 in one dimension.
Looking ahead, the Christoffel symbol Γijk\Gamma_{ij}^{k} will be defined as the contravariant coefficients of Γij\mathbf{\Gamma}_{ij}, i.e.
Γij=ΓijkZk.(12.20)\mathbf{\Gamma}_{ij}=\Gamma_{ij}^{k}\mathbf{Z}_{k}. \tag{12.20}
Before we get there, however, let us visualize the vectors Γij\mathbf{\Gamma }_{ij} in polar coordinates. This will later enable us to establish the values of Γijk\Gamma_{ij}^{k} in all the common coordinate systems.

12.2.1The vector Γ11\mathbf{\Gamma}_{11}

Let us begin with the vector
Γ11=Z1Z1.(12.7)\mathbf{\Gamma}_{11}=\frac{\partial\mathbf{Z}_{1}}{\partial Z^{1}}.\tag{12.7}
Recall that Z1\mathbf{Z}_{1} is the unit vector pointing in the radial direction away from the origin. Therefore, the vector Z1\mathbf{Z}_{1} remains constant as the coordinate Z1Z^{1}, i.e. rr, changes, as illustrated in the following figure:
(12.8)
Therefore, we conclude that Z1/Z1\partial\mathbf{Z}_{1}/\partial Z^{1} vanishes, i.e.
Γ11=0.(12.9)\mathbf{\Gamma}_{11}=\mathbf{0.}\tag{12.9}

12.2.2The vector Γ12=Γ21\mathbf{\Gamma}_{12}=\mathbf{\Gamma}_{21}

We will now calculate both
Γ12=Z1Z2    and     Γ21=Z2Z1(12.10)\mathbf{\Gamma}_{12}=\frac{\partial\mathbf{Z}_{1}}{\partial Z^{2}}\text{ \ \ \ and \ \ \ \ }\mathbf{\Gamma}_{21}=\frac{\partial\mathbf{Z}_{2}}{\partial Z^{1}}\tag{12.10}
and confirm that the two vectors are equal. Let us begin with Γ12\mathbf{\Gamma }_{12}. As Z2Z^{2}, i.e. θ\theta, increases, the outward unit vector Z1\mathbf{Z}_{1} rotates counterclockwise.
(12.11)
We have studied this very vector-valued function on a number of occasions and know that its derivative is the unit vector counterclockwise orthogonal to Z1\mathbf{Z}_{1}.
Let us now turn our attention to Γ21\mathbf{\Gamma}_{21}. Recall that Z2\mathbf{Z}_{2} is a vector of length rr that is counterclockwise orthogonal to Z1\mathbf{Z}_{1}. As the coordinate Z1Z^{1}, i.e. rr, increases, the length of the Z2\mathbf{Z}_{2} increases and, in fact, equals rr, while its direction remains constant.
(12.12)
Thus, Γ21\mathbf{\Gamma}_{21} is a unit vector in the same direction, i.e. counterclockwise orthogonal to Z1\mathbf{Z}_{1}. As expected, the two calculations yielded the same result!
Notice that in describing the vector Γ21=Γ12\mathbf{\Gamma}_{21}=\mathbf{\Gamma }_{12} as the unit vector in the direction counterclockwise orthogonal to Z1\mathbf{Z}_{1}, we used pure geometric terms. However, since we now have the covariant basis Zi\mathbf{Z}_{i} at our disposal, we are also able to describe the same vector analytically by giving the expressions for its contravariant components. Since Γ21=Γ12\mathbf{\Gamma}_{21}=\mathbf{\Gamma} _{12} points in the same direction as Z2\mathbf{Z}_{2} and has length 11 (while the length of Z2\mathbf{Z}_{2} is rr), we have
Γ21=Γ12=1rZ2.(12.13)\mathbf{\Gamma}_{21}=\mathbf{\Gamma}_{12}=\frac{1}{r}\mathbf{Z}_{2}\mathbf{.}\tag{12.13}

12.2.3The vector Γ22\mathbf{\Gamma}_{22}

Finally, we turn our attention to
Γ22=Z2Z2.(12.14)\mathbf{\Gamma}_{22}=\frac{\partial\mathbf{Z}_{2}}{\partial Z^{2}}.\tag{12.14}
As the coordinate Z2Z^{2}, i.e. θ\theta, increases, Z2\mathbf{Z}_{2} rotates counterclockwise while maintaining its length of rr.
(12.15)
This is once again an evolution we are quite familiar with and can readily conclude that Γ22\mathbf{\Gamma}_{22} is a vector of length rr that is counterclockwise orthogonal to Z2\mathbf{Z}_{2}.
In order to give the analytical expressions for the contravariant components of Γ22\mathbf{\Gamma}_{22}, as we did for Γ12=Γ21\mathbf{\Gamma}_{12}=\mathbf{\Gamma }_{21}, note that Γ22\mathbf{\Gamma}_{22} points in the direction opposite to Z1\mathbf{Z}_{1}. Since the length of Γ22\mathbf{\Gamma}_{22} is rr (while the length of Z1\mathbf{Z}_{1} is 11), we have
Γ22=rZ1.(12.16)\mathbf{\Gamma}_{22}=-r\mathbf{Z}_{1}.\tag{12.16}

12.2.4Summary

Let us summarize our findings by arranging the analytical expressions for the vectors Γij\mathbf{\Gamma}_{ij} in a 2×22\times2 matrix:
[Γ11Γ12Γ21Γ22]= [01rZ21rZ2rZ1].(12.17)\left[ \begin{array} {cc} \mathbf{\Gamma}_{11} & \mathbf{\Gamma}_{12}\\ \mathbf{\Gamma}_{21} & \mathbf{\Gamma}_{22} \end{array} \right] =\text{ }\left[ \begin{array} {cc} \mathbf{0} & \frac{1}{r}\mathbf{Z}_{2}\\ \frac{1}{r}\mathbf{Z}_{2} & -r\mathbf{Z}_{1} \end{array} \right] .\tag{12.17}

12.3.1An implicit definition

In the preceding Section, we established the analytical expressions for the vectors
Γij=Zi(Z)Zj.(12.2)\mathbf{\Gamma}_{ij}=\frac{\partial\mathbf{Z}_{i}\left( Z\right) }{\partial Z^{j}}. \tag{12.2}
in polar coordinates. More specifically, we determined the contravariant components of Γij\mathbf{\Gamma}_{ij}, i.e. components with respect to the covariant basis Zi\mathbf{Z}_{i}. When a single vector U\mathbf{U} is decomposed with respect to the covariant basis, the resulting contravariant components UiU^{i} form a first-order system. When each vector in a first-order system Ui\mathbf{U}_{i} is decomposed with respect to the covariant basis, the resulting components UijU_{i}^{j}, where
Ui=UijZj,(12.18)\mathbf{U}_{i}=U_{i}^{j}\mathbf{Z}_{j},\tag{12.18}
form a second-order system. When each vector in a second-order system Uij\mathbf{U}_{ij} is decomposed with respect to the covariant basis, the contravariant components UijkU_{ij}^{k}, where
Uij=UijkZk,(12.19)\mathbf{U}_{ij}=U_{ij}^{k}\mathbf{Z}_{k},\tag{12.19}
form a third-order system.
The Christoffel symbol Γijk\Gamma_{ij}^{k} is precisely that for the vectors Γij\mathbf{\Gamma}_{ij}, i.e. the third-order system that consists of contravariant components of Γij\mathbf{\Gamma}_{ij}. In other words, the Christoffel symbol Γijk\Gamma_{ij}^{k} is defined by the identity
ZiZj=ΓijkZk.(12.20)\frac{\partial\mathbf{Z}_{i}}{\partial Z^{j}}=\Gamma_{ij}^{k}\mathbf{Z}_{k}.\tag{12.20}
Since Γij\mathbf{\Gamma}_{ij} is symmetric, i.e.
Γij=Γji,(12.5)\mathbf{\Gamma}_{ij}=\mathbf{\Gamma}_{ji}, \tag{12.5}
the Christoffel symbol Γijk\Gamma_{ij}^{k} is symmetric in its subscripts:
Γijk=Γjik.(12.21)\Gamma_{ij}^{k}=\Gamma_{ji}^{k}.\tag{12.21}
In the nn-dimensional space, Γijk\Gamma_{ij}^{k} has n3n^{3} elements. However, because of the above symmetry, only n2(n+1)/2n^{2}\left( n+1\right) /2 entries can be distinct, i.e. 1818 in three dimensions, 66 in two dimensions, and 11 in one dimension. In special coordinate systems, the Christoffel symbol Γijk\Gamma_{ij}^{k} typically has only a few nonzero elements, so much so that it is usually more efficient to describe Γijk\Gamma_{ij}^{k} by listing its few nonzero elements. For example, the Christoffel symbol in polar coordinates can be summarized as follows:
Γ221=r    and    Γ122=Γ212=1r.(12.22)\Gamma_{22}^{1}=-r\text{\ \ \ \ and \ \ \ }\Gamma_{12}^{2}=\Gamma_{21} ^{2}=\frac{1}{r}.\tag{12.22}

12.3.2The order of the indices in Γijk\Gamma_{ij}^{k}

We have mentioned previously that, in order to avoid potential ambiguities, it is often necessary to agree on the order of indices. For the Christoffel symbol Γijk\Gamma_{ij}^{k}, two different conventions are found in the available texts. According to one, the superscript is treated as the first index and, according to the other, as the last. We will follow Hermann Weyl's Space Time Matter, and treat the superscript as the first index and the subscripts as second and third. We could denote the Christoffel symbol by the symbol Γijk\Gamma_{\cdot ij}^{k} with a dot placeholder to make this choice explicit. However, we will prefer to rely on the stated convention rather than the placeholder.
In the absence of the convention and the dot placeholder, the result of lowering the superscript, denoted, say, by Γrst\Gamma_{rst}, would be ambiguous since we would not know which of the indices is the lowered superscript. Thanks to the convention, on the other hand, we know that it is the index rr. Nevertheless, even when the ordering of the indices is clarified by a convention, it is customary to separate the subscripts by a comma, as in
Γk,ij=ZklΓijl(12.23)\Gamma_{k,ij}=Z_{kl}\Gamma_{ij}^{l}\tag{12.23}
Some sources refer to Γk,ij\Gamma_{k,ij} as the Christoffel symbol of the first kind and Γijk\Gamma_{ij}^{k} as the Christoffel symbol of the second kind. However, we see no need to make this distinction since we treat systems related by index juggling as different manifestations of the same objects.

12.3.3An explicit expression for the Christoffel symbol

The equation
Γij=ΓijkZk,(12.20)\mathbf{\Gamma}_{ij}=\Gamma_{ij}^{k}\mathbf{Z}_{k}, \tag{12.20}
where
Γij=ZiZj,(12.2)\mathbf{\Gamma}_{ij}=\frac{\partial\mathbf{Z}_{i}}{\partial Z^{j}}, \tag{12.2}
uniquely defines the Christoffel symbol Γijk\Gamma_{ij}^{k} as the contravariant components of Γij\mathbf{\Gamma}_{ij}. However, the equation
Γij=ΓijkZk,(12.20)\mathbf{\Gamma}_{ij}=\Gamma_{ij}^{k}\mathbf{Z}_{k}, \tag{12.20}
does not provide an explicit analytical expression for Γijk\Gamma _{ij}^{k}. Of course, such an expression is readily available with the help of the dot product. In Chapter 10, we established that the contravariant components UkU^{k} of a vector U\mathbf{U} are given by the dot product with the contravariant basis element Zk\mathbf{Z}^{k} with U\mathbf{U}:
Uk=ZkU.(12.24)U^{k}=\mathbf{Z}^{k}\cdot\mathbf{U.}\tag{12.24}
Applying this formula to the vector
Γij=ZiZj,(12.2)\mathbf{\Gamma}_{ij}=\frac{\partial\mathbf{Z}_{i}}{\partial Z^{j}}, \tag{12.2}
we find
Γijk=ZkZiZj.(12.25)\Gamma_{ij}^{k}=\mathbf{Z}^{k}\cdot\frac{\partial\mathbf{Z}_{i}}{\partial Z^{j}}.\tag{12.25}
This identity will feature prominently in many future analyses.
An application of the product rule to the dot product on the right of the above identity leads to another insightful expression for the Christoffel symbol Γijk\Gamma_{ij}^{k}. Using the product rule in the form fg=(fg)fgfg^{\prime }=\left( fg\right) ^{\prime}-f^{\prime}g, we find
Γijk=(ZkZi)ZjZkZjZi.(12.26)\Gamma_{ij}^{k}=\frac{\partial\left( \mathbf{Z}^{k}\cdot\mathbf{Z} _{i}\right) }{\partial Z^{j}}-\frac{\partial\mathbf{Z}^{k}}{\partial Z^{j} }\cdot\mathbf{Z}_{i}.\tag{12.26}
Since the dot product ZkZi\mathbf{Z}^{k}\cdot\mathbf{Z}_{i} equals δik\delta _{i}^{k}, i.e. a system whose elements do not change from one point to another, the first term on the right vanishes. Switching the order of the vectors in the second term, we conclude that Γijk\Gamma_{ij}^{k} is also given by the dot product
Γijk=ZiZkZj.(12.27)\Gamma_{ij}^{k}=-\mathbf{Z}_{i}\cdot\frac{\partial\mathbf{Z}^{k}}{\partial Z^{j}}.\tag{12.27}
This identity shows that the covariant components of the vectors Zk/Zj\partial\mathbf{Z}^{k}/\partial Z^{j} are given by Γijk-\Gamma_{ij}^{k}, i.e.
ZkZj=ΓijkZi.(12.28)\frac{\partial\mathbf{Z}^{k}}{\partial Z^{j}}=-\Gamma_{ij}^{k}\mathbf{Z}^{i}.\tag{12.28}
Thus, the elements of the Christoffel symbol Γijk\Gamma_{ij}^{k} are simultaneously the contravariant components of
ZiZj(12.29)\frac{\partial\mathbf{Z}_{i}}{\partial Z^{j}}\tag{12.29}
and minus the covariant components of
ZkZj.(12.30)\frac{\partial\mathbf{Z}^{k}}{\partial Z^{j}}.\tag{12.30}

12.3.4The tensor notation as a guide for forming expressions

The introduction of the Christoffel symbol provides us with another opportunity to discuss a number of positive aspects of the tensor notation.
The Christoffel symbol Γijk\Gamma_{ij}^{k} is a system of order three -- the highest order of any system we have considered so far. You may feel like the indicial complexity may be beginning to get out of control and that Cartan's proverbial orgies of indices are beginning to obscure the simple geometric picture. You may also think that identities, such as Zi/Zj=ΓijkZk\partial\mathbf{Z}_{i}/\partial Z^{j}=\Gamma_{ij}^{k}\mathbf{Z}_{k} are difficult to remember. In this Section, we will demonstrate that the complexity remains completely under control and that identities such as Zi/Zj=ΓijkZk\partial\mathbf{Z}_{i}/\partial Z^{j}=\Gamma_{ij}^{k}\mathbf{Z}_{k} are not only easy to remember but, in fact, practically write themselves!
Consider the derivative
ZlZm,(12.31)\frac{\partial\mathbf{Z}_{l}}{\partial Z^{m}},\tag{12.31}
where we have purposefully changed the names of the indices in order to give ourselves a fresh start. We will now demonstrate how to recreate the expression on the right featuring the Christoffel symbol simply by following the logic of the tensor notation.
You will certainly remember that this expression involves the Christoffel symbol -- but in what combination? When you inspect the expression Zl/Zm\partial\mathbf{Z}_{l}/\partial Z^{m}, you will notice that it has two subscripts: one from Zl\mathbf{Z}_{l} and the other from ZmZ^{m} being in the "denominator". Thus, these two subscripts will be matched up with the two subscripts of the Christoffel symbol. If the Christoffel symbol was not symmetric in its superscripts, you would need to remember whether you need Γlm\Gamma_{lm} or Γml\Gamma_{ml}. Fortunately, it is symmetric so we do not need to worry about the order of the subscripts.
Thus, we have so far
ZlZm=Γlm(12.32)\frac{\partial\mathbf{Z}_{l}}{\partial Z^{m}}=\mathbf{\Gamma}_{lm}\tag{12.32}
The Christoffel symbol is missing its superscript. We have no choice but to place it there; let us name it nn and pair it up with a covariant basis Zn\mathbf{Z}_{n}, i.e.
ZlZm=ΓlmnZn.(12.33)\frac{\partial\mathbf{Z}_{l}}{\partial Z^{m}}=\Gamma_{lm}^{n}\mathbf{Z}_{n}.\tag{12.33}
The Christoffel symbol Γijk\Gamma_{ij}^{k} captures the rate of change of the covariant basis Zi\mathbf{Z}_{i} with respect to the coordinates ZjZ^{j}. Since the covariant metric tensor ZijZ_{ij} is built up from the covariant basis Zl\mathbf{Z}_{l}, we should be able to calculate its rate of change in terms of the Christoffel symbol.
Recall the definition of the metric tensor ZijZ_{ij}
Zij=ZiZj.(12.34)Z_{ij}=\mathbf{Z}_{i}\cdot\mathbf{Z}_{j}.\tag{12.34}
Differentiating both sides, we find
ZijZk=ZiZkZj+ZiZjZk.(12.35)\frac{\partial Z_{ij}}{\partial Z^{k}}=\frac{\partial\mathbf{Z}_{i}}{\partial Z^{k}}\cdot\mathbf{Z}_{j}+\mathbf{Z}_{i}\cdot\frac{\partial\mathbf{Z}_{j} }{\partial Z^{k}}.\tag{12.35}
Each of the partial derivatives on the right side can be expressed in terms of the Christoffel symbol, i.e.
ZiZk=ΓiklZl and ZjZk=ΓjklZl.(12.36)\frac{\partial\mathbf{Z}_{i}}{\partial Z^{k}}=\Gamma_{ik}^{l}\mathbf{Z} _{l}\text{ and }\frac{\partial\mathbf{Z}_{j}}{\partial Z^{k}}=\Gamma_{jk} ^{l}\mathbf{Z}_{l}.\tag{12.36}
Thus,
ZijZk=ΓiklZlZj+ZiΓjklZl.(12.37)\frac{\partial Z_{ij}}{\partial Z^{k}}=\Gamma_{ik}^{l}\mathbf{Z}_{l} \cdot\mathbf{Z}_{j}+\mathbf{Z}_{i}\cdot\Gamma_{jk}^{l}\mathbf{Z}_{l}.\tag{12.37}
Since ZlZj=Zjl\mathbf{Z}_{l}\cdot\mathbf{Z}_{j}=Z_{jl} and ZiZl=Zil\mathbf{Z}_{i} \cdot\mathbf{Z}_{l}=Z_{il},
ZijZk=ZjlΓikl+ZilΓjkl.(12.38)\frac{\partial Z_{ij}}{\partial Z^{k}}=Z_{jl}\Gamma_{ik}^{l}+Z_{il}\Gamma _{jk}^{l}.\tag{12.38}
This result has a slightly better form when the two terms are switched:
ZijZk=ZilΓjkl+ZjlΓikl.(12.39)\frac{\partial Z_{ij}}{\partial Z^{k}}=Z_{il}\Gamma_{jk}^{l}+Z_{jl}\Gamma _{ik}^{l}.\tag{12.39}
Finally, absorbing the metric tensor into the Christoffel symbol, we find
ZijZk=Γi,jk+Γj,ik.(12.40)\frac{\partial Z_{ij}}{\partial Z^{k}}=\Gamma_{i,jk}+\Gamma_{j,ik}.\tag{12.40}
The identity
ZijZk=Γi,jk+Γj,ik(12.40)\frac{\partial Z_{ij}}{\partial Z^{k}}=\Gamma_{i,jk}+\Gamma_{j,ik} \tag{12.40}
is not the least bit surprising. Since the metric tensor ZijZ_{ij} can be expressed in terms of the covariant basis Zi\mathbf{Z}_{i}, we fully expected to find the expression for the derivatives of the former, i.e. Zij/Zk\partial Z_{ij}/\partial Z^{k}, in terms of the derivatives of the latter, i.e. the Christoffel symbol. What may be at least somewhat surprising is that this relationship can be reversed: the Christoffel symbol can be expressed in terms of the derivatives of the metric tensor.{}
To remove the sense of surprise, let us think of the identity
ZijZk=Γi,jk+Γj,ik(12.40)\frac{\partial Z_{ij}}{\partial Z^{k}}=\Gamma_{i,jk}+\Gamma_{j,ik} \tag{12.40}
as representing equations in which the elements of the Christoffel symbol Γi,jk\Gamma_{i,jk} are the unknowns, and let us do a simple count of equations and the unknowns. Since it has three free indices ii, jj, and kk, the above equation represents n3n^{3} equations in an nn-dimensional space, which matches the number of the elements in a Christoffel symbol. The available symmetries reduce the system to n2(n+1)/2n^{2}\left( n+1\right) /2 equations with n2(n+1)/2n^{2}\left( n+1\right) /2 unknowns: 1818 in three dimensions, 66 in two dimensions, and 11 in one dimension. Thus, expressing the Christoffel symbol in terms of the derivatives of the metric tensor is simply a matter of solving a linear system of equations.
An effective approach to finding the solution relies on a creative manipulation of indices. From the identity
ZijZk=Γi,jk+Γj,ik   ,(12.40)\frac{\partial Z_{ij}}{\partial Z^{k}}=\Gamma_{i,jk}+\Gamma_{j,ik}\ \ \ , \tag{12.40}
obtain equivalent forms by cycling through the index names. For the first variation, rename iji\rightarrow j, jkj\rightarrow k, kik\rightarrow i. For the second variation, perform the very same renaming on the first variation. We end up with the following three equivalent identities:
ZijZk=Γi,jk+Γj,ik          (12.41)ZjkZi=Γj,ki+Γk,ji          (12.42)ZkiZj=Γk,ij+Γi,kj          (12.43)\begin{aligned}\frac{\partial Z_{ij}}{\partial Z^{k}} & =\Gamma_{i,jk}+\Gamma_{j,ik}\ \ \ \ \ \ \ \ \ \ \left(12.41\right)\\\frac{\partial Z_{jk}}{\partial Z^{i}} & =\Gamma_{j,ki}+\Gamma_{k,ji}\ \ \ \ \ \ \ \ \ \ \left(12.42\right)\\\frac{\partial Z_{ki}}{\partial Z^{j}} & =\Gamma_{k,ij}+\Gamma_{i,kj}\ \ \ \ \ \ \ \ \ \ \left(12.43\right)\end{aligned}
The orgy of indices is on full display now! The Christoffel symbols in the above equations all have different combinations of indices. However, note that
Γi,jk=Γi,kj,   Γj,ik=Γj,ki,   and Γk,ij=Γk,ji.(12.44)\Gamma_{i,jk}=\Gamma_{i,kj},\ \ \ \Gamma_{j,ik}=\Gamma_{j,ki},\ \ \ \text{and }\Gamma_{k,ij}=\Gamma_{k,ji}.\tag{12.44}
Sort all commuting indices in alphabetical order in every term of the system
ZijZk=Γi,jk+Γj,ik          (12.45)ZjkZi=Γj,ik+Γk,ij          (12.46)ZikZj=Γk,ij+Γi,jk   ,          (12.47)\begin{aligned}\frac{\partial Z_{ij}}{\partial Z^{k}} & =\Gamma_{i,jk}+\Gamma_{j,ik}\ \ \ \ \ \ \ \ \ \ \left(12.45\right)\\\frac{\partial Z_{jk}}{\partial Z^{i}} & =\Gamma_{j,ik}+\Gamma_{k,ij}\ \ \ \ \ \ \ \ \ \ \left(12.46\right)\\\frac{\partial Z_{ik}}{\partial Z^{j}} & =\Gamma_{k,ij}+\Gamma_{i,jk}\ \ \ ,\ \ \ \ \ \ \ \ \ \ \left(12.47\right)\end{aligned}
and notice that we are now able to isolate Γi,jk\Gamma_{i,jk} by adding the first and the third equations and subtracting the second equation, i.e.
2Γi,jk=ZijZk+ZikZjZjkZi.(12.48)2\Gamma_{i,jk}=\frac{\partial Z_{ij}}{\partial Z^{k}}+\frac{\partial Z_{ik} }{\partial Z^{j}}-\frac{\partial Z_{jk}}{\partial Z^{i}}.\tag{12.48}
Thus,
Γi,jk=12(ZijZk+ZikZjZjkZi).(12.49)\Gamma_{i,jk}=\frac{1}{2}\left( \frac{\partial Z_{ij}}{\partial Z^{k}} +\frac{\partial Z_{ik}}{\partial Z^{j}}-\frac{\partial Z_{jk}}{\partial Z^{i} }\right) .\tag{12.49}
Raising the subscript ii on both sides of the equation yields for the Christoffel symbol in the form Γjki\Gamma_{jk}^{i}, i.e.
Γjki=12Zim(ZmjZk+ZmkZjZjkZm).(12.50)\Gamma_{jk}^{i}=\frac{1}{2}Z^{im}\left( \frac{\partial Z_{mj}}{\partial Z^{k}}+\frac{\partial Z_{mk}}{\partial Z^{j}}-\frac{\partial Z_{jk}}{\partial Z^{m}}\right) .\tag{12.50}
This result will prove crucial when we begin to develop Riemannian spaces and this identity will be adopted as the definition of the Christoffel symbol. Note that we, too, could have adopted this identity as the definition of the Christoffel symbol and, from it, derive all of the other identities involving the Christoffel symbol. This approach to defining the Christoffel symbol is known as intrinsic.
The elements of the Christoffel symbol Γijk\Gamma_{ij}^{k} in all of the most common special coordinate systems can be derived by the approach outlined above in Section 12.2. In this Section, we document those values and leave their calculation as an exercise.

12.6.1In affine coordinates

Since the covariant basis Zi\mathbf{Z}_{i} does not vary from one point to another in affine coordinates, the Christoffel symbol ZijkZ_{ij}^{k} vanishes at all points:
Γijk=0.(12.51)\Gamma_{ij}^{k}=0.\tag{12.51}

12.6.2In cylindrical coordinates

The nonzero elements of the Christoffel symbol are the same as those for polar coordinates derived in Section 12.3:
Γ221=r          (12.52)Γ122=Γ212=1r.          (12.53)\begin{aligned}\Gamma_{22}^{1} & =-r\ \ \ \ \ \ \ \ \ \ \left(12.52\right)\\\Gamma_{12}^{2} & =\Gamma_{21}^{2}=\frac{1}{r}.\ \ \ \ \ \ \ \ \ \ \left(12.53\right)\end{aligned}

12.6.3In spherical coordinates

In spherical coordinates, the nonzero elements of the Christoffel symbol are
Γ221=r          (12.54)Γ331=rsin2θ          (12.55)Γ122=Γ212=1r          (12.56)Γ332=sinθcosθ          (12.57)Γ133=Γ313=1r          (12.58)Γ233=Γ323=1tanθ.          (12.59)\begin{aligned}\Gamma_{22}^{1} & =-r\ \ \ \ \ \ \ \ \ \ \left(12.54\right)\\\Gamma_{33}^{1} & =-r\sin^{2}\theta\ \ \ \ \ \ \ \ \ \ \left(12.55\right)\\\Gamma_{12}^{2} & =\Gamma_{21}^{2}=\frac{1}{r}\ \ \ \ \ \ \ \ \ \ \left(12.56\right)\\\Gamma_{33}^{2} & =-\sin\theta\cos\theta\ \ \ \ \ \ \ \ \ \ \left(12.57\right)\\\Gamma_{13}^{3} & =\Gamma_{31}^{3}=\frac{1}{r}\ \ \ \ \ \ \ \ \ \ \left(12.58\right)\\\Gamma_{23}^{3} & =\Gamma_{32}^{3}=\frac{1}{\tan\theta}.\ \ \ \ \ \ \ \ \ \ \left(12.59\right)\end{aligned}
Deriving these expressions is left as an exercise.
Let us now illustrate how the Christoffel symbol enters analytical calculations. For this demonstration we will return to the analysis of a material particle moving along a trajectory given by the equation
Zi=Zi(t),(10.36)Z^{i}=Z^{i}\left( t\right) , \tag{10.36}
where the Christoffel symbol will appear in the expression for acceleration.

12.7.1A brief review

In Chapter 10, we learned that the contravariant components Vi(t)V^{i}\left( t\right) of the velocity vector V(t)\mathbf{V}\left( t\right) are given by
Vi(t)=dZi(t)dt.(10.37)V^{i}\left( t\right) =\frac{dZ^{i}\left( t\right) }{dt}. \tag{10.37}
Let us remind ourselves of the simple derivation that yielded this identity. If the position vector function R(t)\mathbf{R}\left( t\right) describes the trajectory of the moving particle, then R(t)\mathbf{R}\left( t\right) is given by the composition of the function R(Z)\mathbf{R}\left( Z\right) , i.e. R(Z1,Z2,Z3)\mathbf{R}\left( Z^{1},Z^{2},Z^{3}\right) , with the equations of the motion Zi(t)Z^{i}\left( t\right) :
R(t)=R(Z(t)).(12.60)\mathbf{R}\left( t\right) =\mathbf{R}\left( Z\left( t\right) \right) .\tag{12.60}
Since
V(t)=R(t),(12.61)\mathbf{V}\left( t\right) =\mathbf{R}^{\prime}\left( t\right) ,\tag{12.61}
differentiating both sides of the preceding equation with respect to tt yields
V(t)=R(Z)ZidZi(t)dt,(12.62)\mathbf{V}\left( t\right) =\frac{\partial\mathbf{R}\left( Z\right) }{\partial Z^{i}}\frac{dZ^{i}\left( t\right) }{dt},\tag{12.62}
or
V(t)=dZi(t)dtZi.(12.63)\mathbf{V}\left( t\right) =\frac{dZ^{i}\left( t\right) }{dt}\mathbf{Z} _{i}.\tag{12.63}
Since V=ViZi\mathbf{V}=V^{i}\mathbf{Z}_{i}, we conclude that the components Vi(t)V^{i}\left( t\right) are given by
Vi(t)=dZi(t)dt.(10.37)V^{i}\left( t\right) =\frac{dZ^{i}\left( t\right) }{dt}. \tag{10.37}

12.7.2The derivation of Ai(t)A^{i}\left( t\right)

Let us now turn our attention to the components AiA^{i} of the acceleration vector A\mathbf{A}:
A=AiZi.(12.64)\mathbf{A}=A^{i}\mathbf{Z}_{i}.\tag{12.64}
In affine coordinates, where the covariant basis Zi\mathbf{Z}_{i} does not vary from one point to another, deriving the expression for Ai(t)A^{i}\left( t\right) is an entirely straightforward exercise. Differentiating the identity
V(t)=Vi(t)Zi(12.65)\mathbf{V}\left( t\right) =V^{i}\left( t\right) \mathbf{Z}_{i}\tag{12.65}
with respect to tt yields
V(t)=dVi(t)dtZi.(12.66)\mathbf{V}^{\prime}\left( t\right) =\frac{dV^{i}\left( t\right) } {dt}\mathbf{Z}_{i}.\tag{12.66}
In other words
A(t)=dVi(t)dtZi.(12.67)\mathbf{A}\left( t\right) =\frac{dV^{i}\left( t\right) }{dt}\mathbf{Z} _{i}.\tag{12.67}
Since A=AiZi\mathbf{A}=A^{i}\mathbf{Z}_{i}, the components AiA^{i} in affine coordinates are obtained by simply differentiating the components of velocity with respect to time
Ai(t)=dVi(t)dt.(12.68)A^{i}\left( t\right) =\frac{dV^{i}\left( t\right) }{dt}.\tag{12.68}
This corresponds perfectly to our Cartesian intuition developed by our physics textbooks.
In curvilinear coordinates, however, we must account for the spatial variability of Zi\mathbf{Z}_{i}. In order to acknowledge that variability we must write the equation for V(t)\mathbf{V}\left( t\right) as
V(t)=Vi(t)Zi(t),(12.69)\mathbf{V}\left( t\right) =V^{i}\left( t\right) \mathbf{Z}_{i}\left( t\right) ,\tag{12.69}
where the function Zi(t)\mathbf{Z}_{i}\left( t\right) represents the covariant basis vectors Zi\mathbf{Z}_{i} along the particle's trajectory. Differentiating both sides of this identity with respect to tt yields
A(t)=dVi(t)dtZi(t)+Vi(t)dZi(t)dt.(12.70)\mathbf{A}\left( t\right) =\frac{dV^{i}\left( t\right) }{dt}\mathbf{Z} _{i}\left( t\right) +V^{i}\left( t\right) \frac{d\mathbf{Z}_{i}\left( t\right) }{dt}.\tag{12.70}
Dropping the functional dependence of the terms, we write
A=dVidtZi+VidZidt.(12.71)\mathbf{A}=\frac{dV^{i}}{dt}\mathbf{Z}_{i}+V^{i}\frac{d\mathbf{Z}_{i}}{dt}.\tag{12.71}
Due to the presence of the second term, the identity Ai=dVi/dtA^{i}=dV^{i}/dt is invalid in curvilinear coordinates.
In order to analyze the system dZi(t)/dtd\mathbf{Z}_{i}\left( t\right) /dt, recall that the covariant basis Zi\mathbf{Z}_{i} is defined in the broader ambient space. Thus, Zi(t)\mathbf{Z}_{i}\left( t\right) can be constructed by composing the function Zi(Z)\mathbf{Z}_{i}\left( Z\right) , i.e. Zi(Z1,Z2,Z3)\mathbf{Z} _{i}\left( Z^{1},Z^{2},Z^{3}\right) , with the equations of the motion Zi(t)Z^{i}\left( t\right) :
Zi(t)=Zi(Z(t)).(12.72)\mathbf{Z}_{i}\left( t\right) =\mathbf{Z}_{i}\left( Z\left( t\right) \right) .\tag{12.72}
An application of the chain rule yields
dZidt=Zi(Z)ZjdZj(t)dt.(12.73)\frac{d\mathbf{Z}_{i}}{dt}=\frac{\partial\mathbf{Z}_{i}\left( Z\right) }{\partial Z^{j}}\frac{dZ^{j}\left( t\right) }{dt}.\tag{12.73}
The last term, dZj/dtdZ^{j}/dt is, of course, the velocity component VjV^{j}, so
dZidt=Zi(Z)ZjVj.(12.74)\frac{d\mathbf{Z}_{i}}{dt}=\frac{\partial\mathbf{Z}_{i}\left( Z\right) }{\partial Z^{j}}V^{j}.\tag{12.74}
More interesting, however, is the term Zi(Z)/Zj\partial\mathbf{Z}_{i}\left( Z\right) /\partial Z^{j} which we recognize to be precisely ΓijkZk\Gamma_{ij} ^{k}\mathbf{Z}_{k}. Thus, we arrive at the identity
dZidt=ΓijkVjZk.(12.75)\frac{d\mathbf{Z}_{i}}{dt}=\Gamma_{ij}^{k}V^{j}\mathbf{Z}_{k}.\tag{12.75}
Substituting this result into the identity
A=dVidtZi+VidZidt(12.71)\mathbf{A}=\frac{dV^{i}}{dt}\mathbf{Z}_{i}+V^{i}\frac{d\mathbf{Z}_{i}}{dt} \tag{12.71}
we arrive at the following expression for acceleration:
A=dVidtZi+ΓijkViVjZk.(12.76)\mathbf{A}=\frac{dV^{i}}{dt}\mathbf{Z}_{i}+\Gamma_{ij}^{k}V^{i}V^{j} \mathbf{Z}_{k}.\tag{12.76}
Since our goal is to determine the acceleration component AiA^{i}, we must modify the expression on the right so it appears in the form of a contraction with the covariant basis Zi\mathbf{Z}_{i}. Thus, the covariant basis in the second term must have the subscript ii. In order to achieve this, cycle the names of the indices ijkii\rightarrow j\rightarrow k\rightarrow i to obtain
ΓijkViVjZk=ΓjkiVjVkZi(12.77)\Gamma_{ij}^{k}V^{i}V^{j}\mathbf{Z}_{k}=\Gamma_{jk}^{i}V^{j}V^{k} \mathbf{Z}_{i}\tag{12.77}
and
A=dVidtZi+ΓjkiVjVkZi.(12.78)\mathbf{A}=\frac{dV^{i}}{dt}\mathbf{Z}_{i}+\Gamma_{jk}^{i}V^{j}V^{k} \mathbf{Z}_{i}.\tag{12.78}
We can now factor out Zi\mathbf{Z}_{i}:
A=(dVidt+ΓjkiVjVk)Zi.(12.79)\mathbf{A}=\left( \frac{dV^{i}}{dt}+\Gamma_{jk}^{i}V^{j}V^{k}\right) \mathbf{Z}_{i}.\tag{12.79}
From this form, we conclude that the component AiA^{i} is given by
Ai=dVidt+ΓjkiVjVk.(12.80)A^{i}=\frac{dV^{i}}{dt}+\Gamma_{jk}^{i}V^{j}V^{k}.\tag{12.80}
This formula is an important milestone as it succeeds in expressing the component AiA^{i} of the acceleration in terms of objects that are available in the coordinate space. After all, recall that the identity
Γjki=12Zim(ZmjZk+ZmkZjZjkZm)(12.50)\Gamma_{jk}^{i}=\frac{1}{2}Z^{im}\left( \frac{\partial Z_{mj}}{\partial Z^{k}}+\frac{\partial Z_{mk}}{\partial Z^{j}}-\frac{\partial Z_{jk}}{\partial Z^{m}}\right) \tag{12.50}
tells us that the Christoffel symbol is available in the coordinate space once the metric tensor field has been calculated. Therefore, the equation
Ai=dVidt+ΓjkiVjVk.(12.80)A^{i}=\frac{dV^{i}}{dt}+\Gamma_{jk}^{i}V^{j}V^{k}. \tag{12.80}
demonstrates that the analysis of a moving material particle can be conducted -- at least up to the second derivative -- strictly in the coordinate space without a need for continual reference to the covariant basis Zi\mathbf{Z}_{i} . The term ΓjkiVjVk\Gamma_{jk}^{i}V^{j}V^{k} may be thought of as the correction for the spatial variability of the covariant basis.

12.7.3Example: Uniform circular motion in polar coordinates

In Chapter 10, we calculated the components of the velocity vector of a material particle moving around a circle of radius RR with angular velocity ω\omega in polar coordinates (r,θ)\left( r,\theta\right) . We will now repeat that calculation and then take it a step further by calculating the components of the acceleration.
In polar coordinates Z1=rZ^{1}=r and Z2=θZ^{2}=\theta, the equations of the motion read
Z1(t)=R          (12.81)Z2(t)=ωt          (12.82)\begin{aligned}Z^{1}\left( t\right) & =R\ \ \ \ \ \ \ \ \ \ \left(12.81\right)\\Z^{2}\left( t\right) & =\omega t\ \ \ \ \ \ \ \ \ \ \left(12.82\right)\end{aligned}
Since
Vi=dZidt,(10.37)V^{i}=\frac{dZ^{i}}{dt}, \tag{10.37}
the components ViV^{i} of velocity correspond to
[dZ1dtdZ2dt]=[0ω].(12.83)\left[ \begin{array} {c} \frac{dZ^{1}}{dt}\\ \frac{dZ^{2}}{dt} \end{array} \right] =\left[ \begin{array} {c} 0\\ \omega \end{array} \right] .\tag{12.83}
As we have just derived, the components AiA^{i} of acceleration are given by
Ai=dVidt+ΓjkiVjVk.(12.80)A^{i}=\frac{dV^{i}}{dt}+\Gamma_{jk}^{i}V^{j}V^{k}. \tag{12.80}
Since the velocity components Vi(t)V^{i}\left( t\right) are constants, the only surviving term is ΓjkiVjVk\Gamma_{jk}^{i}V^{j}V^{k}:
Ai=ΓjkiVjVk.(12.84)A^{i}=\Gamma_{jk}^{i}V^{j}V^{k}.\tag{12.84}
Let us fully unpack this identity as follows:
A1=Γ111V1V1+Γ121V1V2+Γ211V2V1+Γ221V2V2          (12.85)A2=Γ112V1V1+Γ122V1V2+Γ212V2V1+Γ222V2V2          (12.86)\begin{aligned}A^{1} & =\Gamma_{11}^{1}V^{1}V^{1}+\Gamma_{12}^{1}V^{1}V^{2}+\Gamma_{21} ^{1}V^{2}V^{1}+\Gamma_{22}^{1}V^{2}V^{2}\ \ \ \ \ \ \ \ \ \ \left(12.85\right)\\A^{2} & =\Gamma_{11}^{2}V^{1}V^{1}+\Gamma_{12}^{2}V^{1}V^{2}+\Gamma_{21} ^{2}V^{2}V^{1}+\Gamma_{22}^{2}V^{2}V^{2}\ \ \ \ \ \ \ \ \ \ \left(12.86\right)\end{aligned}
Since V1=0V^{1}=0 and the only nonvanishing elements of the Christoffel symbol are
Γ122=Γ212=1r, and          (12.87)Γ221=r,          (12.88)\begin{aligned}\Gamma_{12}^{2} & =\Gamma_{21}^{2}=\frac{1}{r}\text{, and}\ \ \ \ \ \ \ \ \ \ \left(12.87\right)\\\Gamma_{22}^{1} & =-r,\ \ \ \ \ \ \ \ \ \ \left(12.88\right)\end{aligned}
the only surviving term is Γ221V2V2\Gamma_{22}^{1}V^{2}V^{2} in A1A^{1} and we find:
A1=Γ221V2V2=ω2R          (12.89)A2=0          (12.90)\begin{aligned}A^{1} & =\Gamma_{22}^{1}V^{2}V^{2}=-\omega^{2}R\ \ \ \ \ \ \ \ \ \ \left(12.89\right)\\A^{2} & =0\ \ \ \ \ \ \ \ \ \ \left(12.90\right)\end{aligned}
which completes our calculation of the components AiA^{i}. We must emphasize that the entire analysis was performed strictly in the coordinate space.
Stepping back into the geometric space, the acceleration vector A\mathbf{A} can be obtained by contracting AiA^{i} with the covariant basis Zi\mathbf{Z} _{i}. The result is the vector
A=ω2RZ1(12.91)\mathbf{A}=-\omega^{2}R\mathbf{Z}_{1}\tag{12.91}
that has a length of ω2R\omega^{2}R and points directly towards the center of the circle. This is a familiar result from elementary Physics textbooks.

12.7.4The jolt of a moving particle

Let us take our analysis a step further and determine the components JiJ^{i} of the jolt J(t)\mathbf{J}\left( t\right) , defined as the derivative of acceleration, i.e.
J(t)=A(t).(12.92)\mathbf{J}\left( t\right) =\mathbf{A}^{\prime}\left( t\right) .\tag{12.92}
It is left as an exercise to show that the components JiJ^{i} are given by the identity
Ji=dAidt+ΓjkiAjVk.(12.93)J^{i}=\frac{dA^{i}}{dt}+\Gamma_{jk}^{i}A^{j}V^{k}.\tag{12.93}

12.7.5The δ/δt\delta/\delta t-derivative

Thanks to the symmetry Γjki=Γkji\Gamma_{jk}^{i}=\Gamma_{kj}^{i} of the Christoffel symbol, the identity
Ji=dAidt+ΓjkiAjVk(12.93)J^{i}=\frac{dA^{i}}{dt}+\Gamma_{jk}^{i}A^{j}V^{k} \tag{12.93}
can be rewritten in the form
Ji=dAidt+VjΓjkiAk.(12.94)J^{i}=\frac{dA^{i}}{dt}+V^{j}\Gamma_{jk}^{i}A^{k}.\tag{12.94}
This form is particularly interesting since it invites the introduction of a new differential operator which we will call the δ/δt\delta/\delta t-derivative, pronounced the delta-by-delta-tt derivative.
The δ/δt\delta/\delta t-derivative applies to first-order time-dependent variants with superscripts defined along the trajectory of the particle. For such a variant Ui(t)U^{i}\left( t\right) and the trajectory given by the equations of the motion
Zi=Zi(t),(10.36)Z^{i}=Z^{i}\left( t\right) , \tag{10.36}
define
δUiδt=dUidt+VjΓjkiUk,(12.95)\frac{\delta U^{i}}{\delta t}=\frac{dU^{i}}{dt}+V^{j}\Gamma_{jk}^{i}U^{k},\tag{12.95}
where, as a reminder, ViV^{i} are the componets of velocity along the trajectory given by the equation
Vi(t)=dZi(t)dt.(10.37)V^{i}\left( t\right) =\frac{dZ^{i}\left( t\right) }{dt}. \tag{10.37}
Note the novel structural aspect of this operator, where applying the δ/δt\delta/\delta t-derivative to any element of the system UiU^{i} involves all other elements of the system since the term VjΓjkiUkV^{j}\Gamma_{jk}^{i}U^{k} engages all of them in a contraction.
With the help of the δ/δt\delta/\delta t-derivative, we can rewrite the equations
Ai=dVidt+ΓjkiVjVk.(12.80)A^{i}=\frac{dV^{i}}{dt}+\Gamma_{jk}^{i}V^{j}V^{k}. \tag{12.80}
and
Ji=dAidt+VjΓjkiAk.(12.94)J^{i}=\frac{dA^{i}}{dt}+V^{j}\Gamma_{jk}^{i}A^{k}. \tag{12.94}
In the more compact forms
Ai=δViδt(12.96)A^{i}=\frac{\delta V^{i}}{\delta t}\tag{12.96}
and
Ji=δAiδt.(12.97)J^{i}=\frac{\delta A^{i}}{\delta t}.\tag{12.97}
In general, for a vector U(t)\mathbf{U}\left( t\right) with components Ui(t)U^{i}\left( t\right) , i.e.
U(t)=Ui(t)Zi(t),(12.98)\mathbf{U}\left( t\right) =U^{i}\left( t\right) \mathbf{Z}_{i}\left( t\right) ,\tag{12.98}
the components of the derivative U(t)\mathbf{U}^{\prime}\left( t\right) are given by δUi(t)/δt\delta U^{i}\left( t\right) /\delta t, i.e.
U(t)=δUi(t)δtZi(t).(12.99)\mathbf{U}^{\prime}\left( t\right) =\frac{\delta U^{i}\left( t\right) }{\delta t}\mathbf{Z}_{i}\left( t\right) .\tag{12.99}
The δ/δt\delta/\delta t-derivative can be extended to first-order variants with covariant indices and, in fact, to variants of arbitrary order and arbitrary indicial signatures. The resulting full-fledged δ/δt\delta/\delta t-derivative has an array of remarkable properties that make it an operator of great utility. However, we will not discuss the development of this operator here for fear that that would steal the thunder of the covariant derivative which we will introduce right after we establish the concept of a tensor in Chapter 14.
If a vector U(t)\mathbf{U}\left( t\right) is constant along the trajectory of a particle, i.e.
U(t)=Constant,(12.100)\mathbf{U}\left( t\right) =\operatorname{Constant},\tag{12.100}
then its components satisfy
δUiδt=0,(12.101)\frac{\delta U^{i}}{\delta t}=0,\tag{12.101}
or, in expanded form,
dUidt+VjΓjkiUk=0.(12.102)\frac{dU^{i}}{dt}+V^{j}\Gamma_{jk}^{i}U^{k}=0.\tag{12.102}
This identity gives us a coordinate-space criterion for determining whether two vectors A\mathbf{A} and B\mathbf{B} at different points in space are equal. In order to apply the criterion, one needs to connect the two points by a smooth trajectory and then interpret the above identity as a system of ordinary differential equations. If t1t_{1} corresponds to the point where A\mathbf{A} is found and t2t_{2} corresponds to the point where B\mathbf{B} is found, then we can solve this system of equations from t1t_{1} to t2t_{2} with the components of A\mathbf{A} as the initial condition. If the resulting components at t2t_{2} coincide with the components of B\mathbf{B}, then A\mathbf{A} and B\mathbf{B} are equal.
Exercise 12.1Show that the sum
Γi,jk+Γj,ik(12.103)\Gamma_{i,jk}+\Gamma_{j,ik}\tag{12.103}
is symmetric in ii and jj.
Exercise 12.2Derive the expression for the derivative of the contravariant metric tensor
ZijZk(12.104)\frac{\partial Z^{ij}}{\partial Z^{k}}\tag{12.104}
in terms of the Christoffel symbol.
Exercise 12.3Derive the values of the Christoffel symbol in each of the special coordinate systems described in Section 12.6.
Exercise 12.4Demonstrate that the components JiJ^{i} of jolt are given by the equation
Ji=dAidt+VjΓjkiAk.(12.93)J^{i}=\frac{dA^{i}}{dt}+V^{j}\Gamma_{jk}^{i}A^{k}. \tag{12.93}
Exercise 12.5Show that
δZiδt=0.(12.105)\frac{\delta\mathbf{Z}^{i}}{\delta t}=\mathbf{0.}\tag{12.105}
Exercise 12.6Confirm that the Riemann-Christoffel identity
ΓjmkZiΓimkZj+ΓinkΓjmnΓjnkΓimn=0,(15.127)\frac{\partial\Gamma_{jm}^{k}}{\partial Z^{i}}-\frac{\partial\Gamma_{im}^{k} }{\partial Z^{j}}+\Gamma_{in}^{k}\Gamma_{jm}^{n}-\Gamma_{jn}^{k}\Gamma _{im}^{n}=0, \tag{15.127}
which will be demonstrated in Chapter 15, holds in polar coordinates.
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