Translation:On the Theory of Relativity II: Fourdimensional Vector Analysis
On the Theory of Relativity. II.
Fourdimensional vector analysis^{[1]};
by A. Sommerfeld.
§ 5. The differential operations of fourdimensional vector analysis.Edit
Instead of Minkowski's general symbol lor (Lorentz operation), we introduce the more specific differential operator
Div, Rot, Grad,
as fourdimensional extensions of the usual operations in ordinary vectorcalculus
div, rot, grad.
The summarizing symbol lor will be preferred (similarly to the Hamiltonian in ordinary vector calculus), when one wants (neglecting the illustrative meaning of the single steps) to symbolically verify the vector formulas. However, since at this place as well as in part I, exactly this geometrical interpretation shall be emphasized, it es recommendable to specialize the symbol lor (depending on its application to six, fourvectors or scalars) in the given way. There, the divergence operation is employed in a dual meaning, as vector divergence and as scalar divergence, so that four fundamental vector operations actually exist in four dimensions, against the three differential operations of ordinary vector calculus. For distinction, I will write the vector divergence by German letters (), the scalar divergence by Latin ones (Div).
We will operate at any place, as if the fourth of our world coordinates xyzl were real (in this connection, see the note on p. 752 of part I). This fiction, as far as I see, nowhere encounters difficulties, it is, on the other hand, an essential presupposition for the simplicity of the geometrical way of expression, according to which we will speak in the following, for example, simply about a perpendicularity instead of a noneuclidean perpendicularity, and it makes it possible to supplement the fourdimensional vector expressions in the closest way to the wellknown threedimensional ones.
The following way traversed by us twice in opposite direction, allows us to see that our list might be complete, and that the results obtained in this way, are by their definition independent of the coordinate system.
a) The scalar divergence. Let be an arbitrarily formed, fourdimensional, and infinitely small section of space^{[2]} in the surrounding of the considered spacetimepoint , the element of the (threedimensional) boundary of , the outer normal to . Let be an arbitrary fourvector, its normal component formed in the sense of equation (7). From the fourvector a scalar magnitude Div emerges, which we define as follows^{[3]}:
(16) 
where the integration with respect to is to be extended over the entire boundary of .
If we choose especially as a fourdimensional parallelepiped with edge lengths dx dy dz dl, then we have
(16a) 
If is the fourdensity defined in (1), then, as it was noticed by Minkowski,
becomes identical with the lefthand side of the continuity equation in ordinary hydrodynamics of compressible fluids (up to the factor ).
b) The vector divergence. While we started under a) with a vector of first kind (fourvector) where we obtained a "vector of zero kind" (scalar), we now start with a vector of second kind (sixvector) and derive a vector of first kind (fourvector) from it. Its component with respect to an arbitrary direction is defined by us in the following way. Let be the threedimensional space extended through the considered spacetimepoint perpendicular to , an infinitely small area of it in the surrounding of , the element of its (twodimensional) boundary; the plane perpendicular to it, unequivocally defined by note 2 on p. 753 and containing both the direction as well as the (outer) normal direction of extended in space , shall be indicated by , and shall denote the component of sixvector (formed in the sense of equation (8)) with respect to this plane. Then, let the component of the vectordivergence of be:
(17) 
where the integration with respect to is related to the whole boundary of .
If we especially choose as direction, as threedimensional parallelepiped (located in space) of border length dy, dz, dl, then it is given by (17):
and somewhat more generally for any of the coordinate directions :
(17a) 
in which instant one of the four derivatives, of course, vanishes due to . The formal agreement of this formation with that in (16a) may motivate us to maintain, despite of the different geometrical meaning, the same name.
If particularly means the sixvector of the field, then, for example, due to (2a) and (2a) it becomes for :
and for :
According to the field equations, the first expression is equal to and the latter equal to , so that the fourdensity directly emerges from the field vector by operation . The first half of the MaxwellLorentz equations, including the electric divergence condition, can thus simply be written:
(18) 
c) The supplement of rotation. We start with a vector of third kind (threedimensional space magnitude, see part I, p. 759), with which we simultaneously consider its supplement (a vector of first kind), denote by us as for distinction, where for example. From that, we derive a vector of second kind, the rotation of or the supplement of the rotation of ; its component with respect to a plane is defined by us as follows: Let be the plane normal to through the considered point , an infinitely small area of in the surrounding of , a boundary element of . The normal space with respect to contains the directions and the direction of the outer normal (drawn within ) with respect to . The component of with respect to this normal space is . Then, let the component of rotation of with respect to plane be:
(19) 
If, for example, is a rectangle with sidelengths dn, ds, where the succession of the directions is the positive one, i.e. the same as that of the axes xyzl, then:
(19a) 
It is in agreement with the following definition for the rotation of a vector of first kind and the earlier equation (4c) for the connection of a sixvector with its supplement, when we also write instead:
(19b) 
By the definition (19) we thus calculate the supplement of rotation with respect to plane for the vector of first kind , or the rotation with respect to its perpendicular plane ; but simultaneously also the rotation for the plane for the vector of third kind , or its supplement for its perpendicular plane .
d) The gradient. It would be in agreement with the things done thus far, to start with a fourdimensional space magnitude , which (as undirected) will have a scalar character, and to derive from it a vector of third kind, which (by its components) shall be taken with respect to an arbitrary space . For that, we would have (in the direction normal to ) to separate an infinitely small, linear area , and the difference as replacement for the degenerated integration over the boundary points of , and eventually to form as component of the emerging vector of third kind:
Instead, we will dually reverse our process by starting with a vector of zero kind , i.e. a scalar magnitude too, and derive from it a vector of first kind, the gradient of , by accordingly defining its component with respect to direction :
(20) 
thus especially its four rightangled components by:
(20a) 
c) Rotation. Now, we start with a vector of first kind and derive from it the vector of second kind, its rotation. We obtain its component with respect to any plane, by separating an area from this plane, then we extend the line integral of around it etc., according to the formula analogous to (19) and (19a,b):
(21) 
Under we shall understand two mutually perpendicular directions located in , so that the rotation from to has the same orientation, as the rotation of around . In the current process we thus directly obtain the rotation of a vector of first kind, instead of its supplement as in c).
A suitable example gives the concept of electrodynamic potential, to whose natural introduction we will resort in the next paragraph at equation (25a), while it is only historically mentioned at this place. Let us combine the vector potential and the scalar potential of the ordinary theory to the "vector potential" , with the components
(21a) 
From it, the field can be calculated by the uniform formula
(21b) 
for example (see (21)):
(21b) 
which summarizes the asymmetric formulas of ordinary theory:
Between the scalar and vector potential, in the ordinary theory one has the complicated condition:
which now simply reads by (16a):
(21c) 
b') The supplement of vector divergence. Starting from a vector of second kind , we derive the component of a vector of third kind with respect to any space , by separating (within ) an infinitely small space section with the twodimensional surface element and the mutually perpendicular direction contained in it. While we formed the normal component of to in b), we now consider the surface integral of the tangential component of , namely:
(22) 
If we especially choose as direction, and as threedimensional parallelepiped in space, then the three surface pairs become parallel to its boundary or zl, ly, yz respectively, and therefore:
(22a) 
For the righthand side we can write by (4b):
by which the chosen denotation and more general are justified with respect to (17a). If means the field vector, we have by (22a) and (2):
similarly for the  and direction and for the axis:
However, these expressions vanish according to the MaxwellLorentz field equations; the second half of these equations, including the magnetic divergence condition, can thus be written:
(18*) 
a') The scalar divergence. Starting from a vector of third kind and its components with respect to the tangential spaces of a fourdimensional space section , one could (from the vector of third kind) eventually derive a scalar magnitude  its divergence  by the definition analogous to a). Due to the mutual interchangeability of the vectors of third and first kind (see the end of § 1), nothing new would emerge with respect to a).
The differential operations considered here, are (by their geometric introduction in which coordinate system were not mentioned at all) independent of the choice of reference frame; their coordinate expressions are thus behaving invariant or covariant with respect to Lorentz transformations. This especially applies to the field equations (18) and (18*). The complicated calculations, by which Lorentz (1895 and 1904) and Einstein (1905) proved their applicability independent from the coordinate system, and by which they had to show the meaning of the transformed field vectors, thus become irrelevant in the system of Minkowski's "world".
§ 6. The integral theorems of Gauss, Stokes, Green in four dimensions.Edit
As one directly obtains (in ordinary vector calculus) the theorems of Gauss and Stokes from the concept of div and rot, and Green's theorem is supplemented to that of Gauss by means of the concept of grad, one also will obtain three integral theorems from the concepts of scalar and vectorial divergence and rotation, which we will denote as theorem of Gauss, GaussStokes, and Stokes; there, the "GaussStokes theorem" stands in the middle between the actual theorem of Gauss and Stokes, in the same way as the concept of vector divergence stands between that of scalar divergence and rotation. The theorem of Green thus follows from the connection of the theorem of Gauss with the concept of gradients.
a) The theorem of Gauss. It reads, when is a fourvector, a fourdimensional space area, its threedimensional boundary with the outer normal :
(23) 
Namely, if one separates the space area into sufficiently small spaceelements , and applies to any of them the same equation (16), then over the boundaries all inner ones are canceled from , since they appear twice with opposite sign, and only the parts of the outer boundary of remain.
In particular let be . If one constructs a tube of lines (lines having everywhere the direction of vector ) and if one cuts the tube at an arbitrary place by a ("plane" or curved) space , then according to the theorem of Gauss, one always obtains the same value of . Herein lies, when means the fourdensity, the independence of charge from the reference system (see I. p. 752).
b) The two forms of the theorem of GaussStokes. Let be a sixvector, an arbitrary (not necessarily "plane") threedimensional space section located within the fourdimensional "world", and the normal upon an element of the same. The boundary of space , which will be a closed twotimes extended surface, be ; the single element we imagine as determined by two mutually perpendicular directions , and the surface element normal to as determined by the directions (perpendicular to ) and (within perpendicular to ). Depending as to whether we project to the surface element normal to , or to itself, we obtain the components or . Then by equations (17) and (22):
(24) 
and
(24*) 
The proof (decomposition of space into sufficiently small elements etc.) is the same as under a).
One can use these two forms of the theorem of GaussStokes, to rewrite Maxwell's differential equations (18) and (18a) in integral form.
For this purpose, one considers a twotimesextended closed surface located in the "world", then puts a threetimes extended space through it, and understands as direction as it was explained above. Then it applies due to (24) and (18) or due to (24*) and (18*):
(24a) 
To emphasize the relation of these formulas to the ordinary integral formulation of Maxwell's equations, we consider two special cases:
1. The surface lies in space. Thus
and we have the known relations:
2. The surface be an infinitely flat cylinder, whose basis in space lies, with the generator (length ), parallel to the axis. Stemming from the mantle of the cylinder, one obtains for the lefthand sides of (24a) (when is measured along the contour of the mantle):
or
On the other hand, if one is taking together the two basisareas of the cylinder, then for those it is , and means the normal (located in space) upon the basisarea. Its contribution is thus
or
where the first integral measures the displacement current traversing the basisarea, the second measures the temporal change of the magnetic forceline number. At the same time
becomes the (up to the factor ) convection current traversing perpendicular to . With respect to the relevant cylindric specialization of the integration area, our surface integrals (24a) therefore go over into the known integral form of Maxwell's equations in ordinary notation:
c) The theorem of Stokes. If means an closed onedimensional convolution (arbitrarily located in the world), a twotimes extended surface limited by , a fourvector, then Stokes' theorem is given as a direct consequence of definition equation (21) in the location and order of directions in the form
(25) 
One can remark, that one cannot speak (even with respect to the ordinary threedimensional formulation of Stokes' theorem), as it usually happens, of the normal component, but of the tangential component of rotation, since rotation is also at that place a vector of second kind. If we had started from the supplement of rotation (see the previous paragraph under c), then we would have obtained equation (25) as well.
If it is particularly about a closed surface , then the boundary curve and thus also the righthand side of (25) vanishes, and thus we have
Accordingly it is given from the second form of GaussStokes' theorem (24*), in which was to be integrated on the righthand side over a closed surface , when we include equal to the rotation of an arbitrary fourvector :
Since this equation applies to any section , we conclude the identical relation
(25a) 
"the vector divergence of the supplement of rotation of an arbitrary fourvector vanishes." This can be simply verified using the coordinate expressions (17a) of the vector divergence and (21) of the rotation.
Equation (25a) simultaneously gives the justification for introducing the electrodynamic potential , which was only historically described in the previous paragraph under c'). Namely, since by approach (21b) , the second of Maxwell's equations according to (25a) is identically satisfied; it only remains to determine , so that it also satisfies the first of Maxwell's equations , which now goes over to:
(25b) 
This fourdimensional vector equation represents the most simple form of Maxwell's theory for vacuum; with its integration, the following paragraph is concerned.
However, by the approach with given , the vector is not completely determined. Namely, if is such a vector, then we obtain in a more general vector, which also satisfies the condition , in case also means a vector of everywhere vanishing rotation. It is, as it simply follows from Stokes' theorem, always representable as gradient of a scalar local function , which itself is given by the line integral , extended from an arbitrary fixed to the previously considered spacetime point. From that it can be recognized, that one still can impose the constrain to the potential
(25c) 
Namely, this gives (for the otherwise completely undetermined function ) the condition:
which we can write (following d)) also as , and which can be integrated by the method of the following paragraph.
A similar reasoning as the one leading to (25a), we append to the first form of GaussStokes' theorem, equation (24). Namely, if it is about a closed threetimes extended spacesection , as it is given as boundary of a fourdimensional spacesection , then its boundary surface vanishes and thus also the righthand side of (24), and we obtain
valid for any closed spacesection . If we thus include instead of in Gauss' theorem (23), then the righthand side of this equation becomes zero as well (here, was the normal with respect to spaceelement , denoted in the previous equation as ) and we have
Since this equation applies to any area , we conclude the identical relation
"the scalar divergence of the vector divergence of an arbitrary sixvector vanishes". This can easily be verified with respect to the coordinate expressions of the scalar and vector divergence (equation (16a) and (17a)).
If in particular means the sixvector of the field again, so that due to the first of Maxwell's equations , then (24b) expresses the continuity condition , about which it was spoken in § 5 under a).
d) The theorem of Green. We use a symbol, already introduced by Cauchy and again used by Poincaré,^{[4]} which has to be applied to a scalar function :
(26) 
This extends the ordinary Laplacian differential expression to four dimensions and thus may be denoted as Laplacian expression again. Its geometricalinvariant nature directly follows from the representation .
If and V are now two scalar local functions of the four variables xyzl, then we have by
a fourvector of special construction. Its scalar divergence, which one can think of as formed by differentiation with respect to coordinates xyzl, then becomes:
namely, the two scalar products are mutually canceled. Thus if we include this special fourvector into the theorem of Gauss (23), then it is given
(27) 
i.e, the exact analogue to the ordinary theorem of Green. It is related to an arbitrary worldsection and its threedimensional boundary . Steadiness of the appearing functions and their first derivations is presupposed as in the other theorems of this paragraph. If it is violated in one worldpoint, then one would have to exclude it from the integration by a threedimensional boundary space , like in the ordinary case, and to supplement the integral over of the righthand side of (27).
This is especially then the case, when is set equal to the fourdimensional analogue of the Newtonian potential :
(27a) 
corresponding to the circumstance, that in four dimensions the mathematical analogue to the Newtonian force would be decreasing by the cube of distance, instead of the square. Here, means the fourdimensional distance of the fixed worldpoint ("reference point") with respect to the variable integration point xyzl. The reference point my lie in the integration area and thus may be surrounded by an infinitely small spherical space (radius ). If we calculate for it the righthand side of (27), then it becomes:
Here, means the value of at the reference point (), if the easily verified theorem^{[5]} is employed, according to which the threedimensional boundary of a fourdimensional sphere of radius 1 is equal to , thus the one of radius is equal to . From (27) it thus follows
(27b) 
On the other hand, it is given from (27) with
(27c) 
If the integration area is extended over the whole infinite space , then we can choose as infinitely great sphere (radius ). To this it applies, similarly as above:
where is the average of on the infinitely distant sphere, and because of (27c)
If both is included in (27b), then it is given
As is vanishing against , it thus becomes
(27d) 
By that, we have to calculate for an arbitrary worldpoint except a constant, when in the whole area of real xyzl is given.
To that, however, a remark has to be made concerning the reality relations. As always, we have implicitly presupposed as real the coordinates as well as , and assumed for example, that is only vanishing at one point . This is not the case anymore if it is considered that , it is rather the case that becomes zero in the real worldcoordinates on a threetimes extended cone. Furthermore, with respect to the actually important tasks, is not given for real, but for negativeimaginary values of , namely in the reference system of xyzl, for all times preceding the time coordinate of the origin. Thus one would have (to be able to apply our formulas) to imagine the given values of the negativeimaginary axis of a complex ()plane (see Fig. 3) as analytically extended with respect to the real axis of that plane, and to extend the integration over these real values of , i.e. over the corresponding values of , in which case only vanishes for , when simultaneously . Instead, we will proceed more easily, by deforming the integration path as in Fig. 3 into a slope surrounding the negativeimaginary axis^{[6]}; the integration in (27d) is then to be understood, so that it is to be led with respect to x y z over all real values, with respect to over this slope, and (27d) represents the value of at time , when for all earlier moments the value of is given. The fourdimensional method proves to be equally fruitful also for these and similar integration tasks, and it allows to solve them quite similar to the calculation of the potential of given masses in ordinary potential theory.
§ 7. Determination of the fourpotential and the electrodynamic force.Edit
The differential equation of the fourpotential, denoted by us as the most simple formulation of Maxwell's theory, reads:
(25b) 
For one of the four rightangled components of we thus have by (17a) and (21b):
for which we can write more easily, by constraint (25c)^{[7]}:
(28) 
Thus we have to solve the following problem of fourdimensional potential theory: We seek a solution of equation for an arbitrary spacetimepoint , when the fourdensity , i.e. the charge and velocity of the considered system, is given for all earlier moments . The solution includes equation (27d) with the slopepath denoted in Fig. 3.
If one includes here for any of the components of , considers equation (28) and suppresses the constant irrelevant for our potential, then it is given
(29) 
This most natural representation of electrodynamic potential in the sense of relativity theory, stems from Herglotz^{[8]}. Factually, this representation of course cannot be distinguished from the older formulas, as long as one remains in the original and and accidentally employed reference system of xyzl.
The integration with respect to can always carried out in (29) as well as in all analogous later formulas by Cauchy's residue theorem. Namely, within the slope of Fig. 3 lies the place where of first order vanishes, thus upon which the integration can be drawn together, namely at the place (see (27a)):
(29a) 
On the other hand, the principally equallyvalid place lies upon the positiveimaginary axis of Fig. 3 and gives no contribution to our slope integration.
Based on the worldline of a certain charge element (see Fig. 4) we denote the point of the worldline, which is cut by a cone constructed at point , with Minkowski as lightpoint of . Its coordinates are unequivocally determined when the charge element never moves at superluminal velocity, and the fourth coordinate can be determined, as previously shown, by equation . As it is known, it says that a light signal emanating from worldpoint , reaches worldpoint (i.e. it reaches the spacepoint at time ).
Thus, if we carry out the integration with respect to by means of residueconstruction, thus the emerging formulas will be related to the lightpoint of . For example, in this way the wellknown formula of retarded potential directly emerge from (29). We only show this for the case of a pointlike charge (of a sufficiently distant reference point).
In this case, one can see in (29) as constant during the integration with respect to x y z, and evaluate this integration. However, to avoid from the beginning the introduction of the arbitrary reference system xyzl, we rather use a natural reference system oriented with respect to the worldline of the point charge. Let (see Fig. 4) be the element of normal space of the worldline, the curve element of the world line. This is connected with Minkowski's proper time , so that
(29b) 
Now one has:
(29c) 
The first of these formulas directly follows from the fact, that the length element and the threedimensional spaceelement are mutually normal. In the second formula, as well as denote a four vector directed with respect to the worldline of the charge at the considered place. It only remains to prove, that the vectors on the righthand and lefthand side of this formula are mutually equal as regards their magnitude. With respect to (29b), , thus the magnitude of the righthand side in question is equal to . On the lefthand side, one thinks as decomposed into components with respect to the worldline and perpendicularly to it. The latter ones vanish, the first one becomes equal to by equation (1) part I, where is the "restdensity", i.e. the density of charge viewed by a comoving observer. Accordingly, becomes equal to the total charge. For the magnitude of the lefthand side of (29c), one also has:
If one substitutes from (29c) into (29), it follows:
the integration with respect to the new variable is, quite equal as the one by in Fig. 3, to be extended on an arbitrary complex, clockwise rotation around the lightpoint , and when calculated by Cauchy's theorem gives^{[9]}:
(29d) 
Here,
(29e) 
means the fourvector from the reference point with respect to the corresponding lightpoint of the charge, the velocity vector of the charge at the lightpoint defined in (29c), and its scalar product in the sense of § 3 A. Equation (29d) represents the invariant notation (in the sense of relativity theory) of the pointpotential law (LiénardWiechert); we return to this in the following paragraphs again.
The field of an arbitrarily moving charge at reference point , can be now obtained by formula (21b)
, for example
If one would like to apply this differentiation in the case of a pointcharge upon the calculated formula (29d), then one would be led to complicated considerations,^{[10]} which stem from the fact, that with a variation of also a variation of the lightpoints is connected. It is much simpler to resort to the original formula (29) and to make the passage to the point charge only at the end. From (29) it is given
and somewhat more general for :
(30) 
We immediately pass to the specific electrodynamic force , by imagining a charge distribution of fourdensity in the surrounding of the reference point , then their component is specified by equation (11) as ; for that, one obtains according to the last formula by using of vector explained in (29e), which at first is not yet related with the lightpoint:
and thus generally:
(30a) 
If one immediately goes over to a point charge again, by means of equations (29c), then its specific force action upon distribution is given by:
If the distribution is also pointlike of total charge , then one is able to form the total force exerted by on . This shall be calculated as comoving force in the sense of in equation (15). Thus, one shall multiply with the space element normal to the worldline of , and shall form . With respect to the second line of (29c) it is given, when means the velocity vector of :
(30b) 
Also here, the integration means a rotation of the complex variable around the lightpoint of ; it can immediately carried out by residueconstruction, where now, since the denominator of second order in vanishes, the development of numerator and denominator is to be taken up to terms of second order. The obvious calculation is neglected at this place and concerning its result we refer to equation (37) of the next paragraph, where it is derived in a probably more illustrative but essentially less simple way than at this place. Compared with the somewhat composed form of equation (37), the integral representation contained in equation (30b) is in any case remarkable due to its particular clarity.
§ 8. The cyclic or hyperbolic motion and the electrodynamic elementary laws.Edit
As the most simple example of accelerated motion we consider the interesting case of "hyperbolic motion" treated recently by M. Born^{[11]}. It represents itself (when one again neglects the imaginary character of the time coordinate in terms of expression and drawing) as "cyclic motion", where the reason for its simplicity lies. We namely investigate this motion under the point of view already indicated by Minkowski^{[12]}, that any accelerated motion can always be approximated by "uniformly accelerated" motion, and from that we arrive at an illustrative derivation of the electrodynamic elementary laws.
The electrical system shall be moving, so that for any of its charge elements it applies:
(31) 
At constant and variable these equations give the worldline of the charge element; at constant and variable they determine the "restform" of charge, i.e. the simultaneous locations of their elements observed by a comoving observer. Fig. 5a represents the relations in the plane with and imagined as real: the worldlines are circles , the restform is projected into the variable radius . Fig. 5b shows, as to how the things are with respect to the imaginary constitution of . If one draws and as real coordinates, and puts , where is a real angel, then the worldlines become equally sided hyperbolas and the restform is given by . The asymptotes under 45° are corresponding to a motion with speed of light , which is approximated by hyperbolic motion for .
By the cyclic nature of our problem, the fourdimensional polar coordinates are given instead of the ordinary coordinates xyzl, whose character is mixed of space and time. If we call the corresponding coordinates of the reference point , then we evidently can choose . This means in the way of expression of Fig. 5a, that we can count the coordinate of the single charge elements starting from the radius vector extending through the reference point, which becomes the axis by that. In the way of expression of Fig. 5b we would have to say, that instead of axes and , we can introduce new "mutually normal" axes and , whose first one is going through and whose last one forms (with the hyperbolic asymptotes) the same angle as (harmonic location of axes against both asymptotes). Also related to these axes, the worldlines are equally sided hyperbolas and are (nonEuclidean) perpendicular upon them. At the same time, wh have for the reference point, thus also or . Thus when we would choose in Fig. 5a, then this means in real terms, that we introduce a new primed instead of , which is relatively moving with respect to the original one, and which we (starting from the other one) define by equation (31) of our polar coordinates . The introduction of the primed axes is, however, excluding superluminal velocities, only possible when the reference point lies in one of the two spacelike quadrants of Fig. 5b (see the note in part I, p. 752), i.e. when in the original coordinates applies, what we want to presuppose. In other cases, i.e. when the reference point lies in one of the timelike quadrants, one only needs to exchange the axes and , without additionally changing something essential.
Also the vectors and are decomposed by us into the components with respect to coordinates , where the fourvector is drawn in the successive locations of the charge elements, the fourvector is drawn in the reference point.
Evidently it is:
Vector namely is directed into the direction of the worldline, thus in the direction of increasing ; as well as was the fourth component in the system (see equation (1), = charge density in space), due to the vector character of , the fourth component in the system are equal to ( = charge density in the comoving space = "rest density" = , see equation (1a) and the explanations to equation (29c) of the previous paragraph). Here, is, according to Gauss' theorem, constant along any worldline (independent of ), it is possibly variable from worldline to worldline. Due to the vector summation immediately carried out, we also will need the components and with respect to the axes oriented by of Fig. 5a (the axes , of Fig. 5b). For any place of the world line:
(31a) 
For the calculation of we use equation (29) and substitute (for the integration variables there) . The slope surrounding the imaginary axis in Fig. 3, is corresponding to an integration in over a corresponding slope, upon which goes back from over zero to , and which clockwise envelopes (as earlier) the lightpoint belonging to any worldline. The passage to the new integration variables happens according to the scheme of ordinary polar coordinates:
(31b) 
with the difference, that the integration with respect to (similar to ) is extended over the mentioned slope.
Of the four components of , two are vanishing; namely due to
Of the two other components and it can be said at first, that they are independent of the coordinate of the reference point, by which the cyclic nature of our problem is expressed. Actually, we could (at any location of the reference point) choose the direction drawn to it as zeroray; in the expressions of (in the direction of the zeroray) and of (perpendicular to it), doesn't occur at all. These components become constant for all points or any circle of Fig. 5a (any hyperbola of Fig. 5b), and vector has a constant magnitude and location against the variable radius . On the other hand, the components in a system of general location are of course independent of , namely due to the general formulas for vector transformation:

At the particular location of the axis as in Fig. 5a (the axis as in Fig. 5b), which is convenient for the following, it additionally becomes , due to .
The component can easily be executed. At first, it is because of (31a,b) and (29):
(32) 
Since is independent (see above) from and , then the integral with respect to is simply:
since it is to be extended around point against the positive rotation sense (see Fig. 3). Thus by (32)
(32a) 
here, means the total charge of the system, obtained by integration of rest density over the restform of the system. On the other hand, by (31a,b) and (30):
(32b) 
The integral with respect to is given, quite similar to above, by residueconstruction:
where for , the values (following from and corresponding to the lightpoint) have to be included:
(32c) 
Thus
(32d) 
For a far distant point, one can view and as approximately constant for all charge elements and execute the threetimes integration, where the total charge of the system emerges. Thus one has for the limiting case:
(33) 
In consequence of Fig. 6 one can easily convince himself, that direction and magnitude of vector are only expressed by the state of motion at lightpoint . For this purpose, we calculate the component of on the one hand with respect to direction perpendicular to the direction of motion at the lightpoint, and on the other hand with respect to the tangent in , which may be determined by the fourvector ; here it is to be noticed, that shall mean the angle belonging to (namely counted from as origin); thus:
in the direction :
in the direction
, however, are represented in the figure by the line , and is the projection of vector from the reference point with respect to the lightpoint upon the motion vector , thus^{[13]}
(33a) 
see part I, § 3 A. Our potential is thus represented in terms of direction and magnitude:
(33b) 
The special character of hyperbolic motion is vanished from (33b), this representation applies to any motion affecting our hyperbolic motion at the lightpoint, and was directly taken above (see (29d)) from our general representation (29) by the passage from one pointcharge and by residueconstruction. As to how the relations are in real terms, is alluded to in Fig. 5b: In the projection of the , plane, the lightpoint (of a parallel drawn through with respect to a hyperbolic asymptote) is cut from the worldline, and it is the resultant from the two real components and parallel to the tangent at the lightpoint.
Skipping the calculation of the field, we have to from by (21b), where we of course choose the required rotations, over which the line integral of must be extended, in the sense of our polar coordinate system (see Fig. 5a right above). While the components of vanish, since and is independent of and , it is given^{[14]} by (21):
(34) 
The field, as well as , is only dependent of the coordinates of the reference point and thus constant on the circles of Fig. 5a (the hyperbolas of 5b). On the other hand, it is of course variable upon the line , since any such line is cut by other hyperbolas for variable in Fig. 5b. Thus, while the field is temporally changing in a spatially fixed point, it is constant in a comoving point. Namely, it has at such a point the character of the electric field throughout. Namely, since the direction has simultaneously the direction of the time axis in the comoving ("primed") system, we have to write in consequence of (2):
(34a) 
For an observer resting in the system, on the other hand, the field has, except the electric one, also an magnetic part.
For distant reference points, to which the electric system appears as pointlike, it is given from (33) and (34)
as well as
From the definition of the lightpoint:
it follows, however, since r, y, z are constant during hyperbolic motion:
thus
as well as
therefore, when the index at is suppressed:
(34b) 
These formulas are the most simple expressions of the field produced by any moving point charge. Namely, by putting the curvature circle (curvature hyperbola) at the worldline of the pointcharge in the lightpoint belonging to our reference point, and by replacing the arbitrary motion by cyclic motion upon the curvature circle, the general case is reduced to our formulas (34b).
These formulas are the most simple expression of the field produced by any moving point charge. Namely, by putting the curvature circle (curvature hyperbola) at the worldline of the pointcharge in the lightpoint belonging to our reference point, and by replacing the arbitrary motion by cyclic motion upon the curvature circle, the general case is reduced to our formulas (34b). The occurrence of the curvature radius , which is connected with the acceleration of motion at the lightpoint (see below), is characteristic. The difference between longitudinal and transverse acceleration is only a difference in the choice of reference frame.
At first, we want to circumscribe the formulas (34b), so that only fourvectors related to the lightpoint occur
is the vector of to , the velocity vector in (see equation (33a)) and the acceleration vector in . In the previous definition (equation (29b)) of by the worldline element , since in our cyclic coordinates applies, it evidently becomes , thus according to equations (31)
consequently is follows:
thus has in the lightpoint the direction of radius and the magnitude .
From these four vectors, the following magnitudes independent of reference frame, can be formed:
and
thus by which the formulas (34b) shall be expressed; here, we notice that the other possible invariants have the following simply values according to the above:
(35) 
the latter is due to the perpendicular location of and . As regards the value of , it was given in equation (33a):
(35a) 
Similarly, according to Fig. 6 it is given as projection of upon
thus
(35b) 
and by division of (35a) and (35b):
(35c) 
If we now consider the fourvector derived from the sixvector (see part I, equation (6a)):
Here, the three bracketed magnitudes or the components of with respect to the directions drawn through , are namely
If we thus add the fourth coordinate with respect to the direction (taken through and perpendicular to ) of the increasing , namely (see Fig. 6), then
The sum of is ; the unit vector in this direction represents itself by the unit vectors in the directions and , which are inclined against that by and respectively:
(36) 
thus
Therefore, is decomposed in two or three fourvectors of directions or , namely
(36a) 
We now pass to the specific electrodynamic force (see § 4), by imagining a charge at reference point , whose magnitude and motion is given by the fourvector . The components of with respect to the coordinatedirections are according to equation (11)
Thus we can vectorially write, when we understand under the mentioned unit vector in the direction extended through
or with respect to (36a):
(36b) 
If we now include the value (36) for , then is decomposed into three portions, a location portions of direction , a velocity and acceleration portions of direction and , namely by using of (35a) and (35c):
(36c) 
By that, the general invariant representation of the specific electrodynamic force is achieved. From it, we go over to the total force , by imagining the total charge as pointlike in . We will calculate it as a "comoving force" (in the sense of equation (15) for ), by considering those values of , which appear simultaneously to an observer comoving with , i.e. integrating over a space perpendicular to the worldline of . On the other hand, when integrating over (as remarked in §4) a result depending on the reference system would be given. Consequently, since has the same meaning as in equation (29c), it is thus given from this equation
and from (36c) we obtain the following three portions of the total electrodynamic force:
(37) 
As above in consequence of (33a), one can notice that the special character of hyperbolic motion is vanished from these formulas (hyperbolic motion only served us to conveniently approximate the motion of at the lightpoint), and more generally that one obtains the same formulas, when is calculated for a quite arbitrary motion of . Indeed, the equations (37) are identical with the result of residueconstruction in equation (30b), about which it was spoken on p. 670.
The equations (37) are of course in agreement with the geometric rule given by Minkowski in § V of "Space and Time", and differ from the expressions originally found by Schwarzschild only by supplementing the fourth "energetic component", which by the way is not unimportant for the following, and in the three remaining "dynamic" components only differs by a factor
, ( = velocity of ),
which stems from the fact, that in the course of forming the total force, Schwarzschild integrated over a space , while we integrated over a space .
§ 9. Remarks on the laws of Coulomb and Newton.Edit
A. Coulomb's law. Equations (37) are applied to the most simple case of electrostatics, i.e. two mutually resting point charges. In the sense of relativity theory, two charges are at rest whose worldlines are two parallel lines. In this case
and thus
(38) 
After cancellation of the accelerationportions, force in (38) is thus composed by a location portion and a velocity portion, which at first is related to a lightpoint, however, it simultaneously has the direction of an arbitrary point of the worldline of or due to the presupposed uniformity. We show, that this velocity portion supplements the location portion exactly to a vector which is directed to the point (simultaneous with ) upon the worldline of . There, simultaneity is evidently to be considered from a reference system moving with velocity , in our case the only reference system naturally defined, and again it will (in passing) constructed by an ordinary (euclidean) perpendicularity.
As already employed many times (see p. 676 and 679), the projection of upon is equal to , and the unit vector in the direction of is equal to , thus with respect to :
The nominator in (38) consequently becomes in terms of the meaning of drawn in Fig. 7:
If one applies the Pythagoras to the "rightangled" triangle , then it is additionally given with :
or
(38a) 
The nominator in (38) thus becomes equal to , so that we can write instead of (38):
(39) 
This is the general invariant expression of Coulomb's law.
If we now introduce the special reference system , whose axis forms with the angle , i.e. in which